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In theoretical physics, topological string theory is a version of string theory. Topological string theory appeared in papers by theoretical physicists, such as Edward Witten and Cumrun Vafa, by analogy with Witten's earlier idea of topological quantum field theory.

Overview

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There are two main versions of topological string theory: the topological A-model and the topological B-model. The results of the calculations in topological string theory generically encode all holomorphic quantities within the full string theory whose values are protected by spacetime supersymmetry. Various calculations in topological string theory are closely related to Chern–Simons theory, Gromov–Witten invariants, mirror symmetry, geometric Langlands Program, and many other topics.

The operators in topological string theory represent the algebra of operators in the full string theory that preserve a certain amount[clarification needed] of supersymmetry. Topological string theory is obtained by a topological twist of the worldsheet description of ordinary string theory: the operators are given different spins. The operation is fully analogous to the construction of topological field theory which is a related concept. Consequently, there are no local degrees of freedom in topological string theory.

Admissible spacetimes

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The fundamental strings of string theory are two-dimensional surfaces. A quantum field theory known as the N = (1,1) sigma model is defined on each surface. This theory consist of maps from the surface to a supermanifold. Physically the supermanifold is interpreted as spacetime and each map is interpreted as the embedding of the string in spacetime.

Only special spacetimes admit topological strings. Classically, one must choose a spacetime such that the theory respects an additional pair of supersymmetries[why?], making the spacetime an N = (2,2) sigma model[further explanation needed]. A particular case of this is if the spacetime is a Kähler manifold and the H-flux is identically equal to zero. Generalized Kähler manifolds can have a nontrivial H-flux.

Topological twist

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Ordinary strings on special backgrounds are never topological[why?]. To make these strings topological, one needs to modify the sigma model via a procedure called a topological twist which was invented by Edward Witten in 1988. The central observation[clarification needed] is that these[which?] theories have two U(1) symmetries known as R-symmetries, and the Lorentz symmetry may be modified by mixing rotations and R-symmetries. One may use either of the two R-symmetries, leading to two different theories, called the A model and the B model. After this twist, the action of the theory is BRST exact[further explanation needed], and as a result the theory has no dynamics. Instead, all observables depend on the topology of a configuration. Such theories are known as topological theories.

Classically this procedure is always possible.[further explanation needed]

Quantum mechanically, the U(1) symmetries may be anomalous, making the twist impossible. For example, in the Kähler case with H = 0[clarification needed] the twist leading to the A-model is always possible but that leading to the B-model is only possible when the first Chern class of the spacetime vanishes, implying that the spacetime is Calabi–Yau[clarification needed]. More generally (2,2) theories have two complex structures and the B model exists when the first Chern classes of associated bundles sum to zero whereas the A model exists when the difference of the Chern classes is zero. In the Kähler case the two complex structures are the same and so the difference is always zero, which is why the A model always exists.

There is no restriction on the number of dimensions of spacetime, other than that it must be even because spacetime is generalized Kähler. However, all correlation functions with worldsheets that are not spheres vanish unless the complex dimension of the spacetime is three, and so spacetimes with complex dimension three are the most interesting. This is fortunate for phenomenology, as phenomenological models often use a physical string theory compactified on a 3 complex-dimensional space. The topological string theory is not equivalent to the physical string theory, even on the same space, but certain[which?] supersymmetric quantities agree in the two theories.

Objects

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A-model

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The topological A-model comes with a target space which is a 6 real-dimensional generalized Kähler spacetime. In the case in which the spacetime is Kähler, the theory describes two objects. There are fundamental strings, which wrap two real-dimensional holomorphic curves. Amplitudes for the scattering of these strings depend only on the Kähler form of the spacetime, and not on the complex structure. Classically these correlation functions are determined by the cohomology ring. There are quantum mechanical instanton effects which correct these and yield Gromov–Witten invariants, which measure the cup product in a deformed cohomology ring called the quantum cohomology. The string field theory of the A-model closed strings is known as Kähler gravity, and was introduced by Michael Bershadsky and Vladimir Sadov in Theory of Kähler Gravity.

In addition, there are D2-branes which wrap Lagrangian submanifolds of spacetime. These are submanifolds whose dimensions are one half that of space time, and such that the pullback of the Kähler form to the submanifold vanishes. The worldvolume theory on a stack of N D2-branes is the string field theory of the open strings of the A-model, which is a U(N) Chern–Simons theory.

The fundamental topological strings may end on the D2-branes. While the embedding of a string depends only on the Kähler form, the embeddings of the branes depends entirely on the complex structure. In particular, when a string ends on a brane the intersection will always be orthogonal, as the wedge product of the Kähler form and the holomorphic 3-form is zero. In the physical string this is necessary for the stability of the configuration, but here it is a property of Lagrangian and holomorphic cycles on a Kahler manifold.

There may also be coisotropic branes in various dimensions other than half dimensions of Lagrangian submanifolds. These were first introduced by Anton Kapustin and Dmitri Orlov in Remarks on A-Branes, Mirror Symmetry, and the Fukaya Category

B-model

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The B-model also contains fundamental strings, but their scattering amplitudes depend entirely upon the complex structure and are independent of the Kähler structure. In particular, they are insensitive to worldsheet instanton effects and so can often be calculated exactly. Mirror symmetry then relates them to A model amplitudes, allowing one to compute Gromov–Witten invariants. The string field theory of the closed strings of the B-model is known as the Kodaira–Spencer theory of gravity and was developed by Michael Bershadsky, Sergio Cecotti, Hirosi Ooguri and Cumrun Vafa in Kodaira–Spencer Theory of Gravity and Exact Results for Quantum String Amplitudes.

The B-model also comes with D(-1), D1, D3 and D5-branes, which wrap holomorphic 0, 2, 4 and 6-submanifolds respectively. The 6-submanifold is a connected component of the spacetime. The theory on a D5-brane is known as holomorphic Chern–Simons theory. The Lagrangian density is the wedge product of that of ordinary Chern–Simons theory with the holomorphic (3,0)-form, which exists in the Calabi–Yau case. The Lagrangian densities of the theories on the lower-dimensional branes may be obtained from holomorphic Chern–Simons theory by dimensional reductions.

Topological M-theory

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Topological M-theory, which enjoys a seven-dimensional spacetime, is not a topological string theory, as it contains no topological strings. However topological M-theory on a circle bundle over a 6-manifold has been conjectured to be equivalent to the topological A-model on that 6-manifold.

In particular, the D2-branes of the A-model lift to points at which the circle bundle degenerates, or more precisely Kaluza–Klein monopoles. The fundamental strings of the A-model lift to membranes named M2-branes in topological M-theory.

One special case that has attracted much interest is topological M-theory on a space with G2 holonomy and the A-model on a Calabi–Yau. In this case, the M2-branes wrap associative 3-cycles. Strictly speaking, the topological M-theory conjecture has only been made in this context, as in this case functions introduced by Nigel Hitchin in The Geometry of Three-Forms in Six and Seven Dimensions and Stable Forms and Special Metrics provide a candidate low energy effective action.

These functions are called "Hitchin functional" and Topological string is closely related to Hitchin's ideas on generalized complex structure, Hitchin system, and ADHM construction etc..

Observables

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The topological twist

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The 2-dimensional worldsheet theory is an N = (2,2) supersymmetric sigma model, the (2,2) supersymmetry means that the fermionic generators of the supersymmetry algebra, called supercharges, may be assembled into a single Dirac spinor, which consists of two Majorana–Weyl spinors of each chirality. This sigma model is topologically twisted, which means that the Lorentz symmetry generators that appear in the supersymmetry algebra simultaneously rotate the physical spacetime and also rotate the fermionic directions via the action of one of the R-symmetries. The R-symmetry group of a 2-dimensional N = (2,2) field theory is U(1) × U(1), twists by the two different factors lead to the A and B models respectively. The topological twisted construction of topological string theories was introduced by Edward Witten in his 1988 paper.[1]

What do the correlators depend on?

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The topological twist leads to a topological theory because the stress–energy tensor may be written as an anticommutator of a supercharge and another field. As the stress–energy tensor measures the dependence of the action on the metric tensor, this implies that all correlation functions of Q-invariant operators are independent of the metric. In this sense, the theory is topological.

More generally, any D-term in the action, which is any term which may be expressed as an integral over all of superspace, is an anticommutator of a supercharge and so does not affect the topological observables. Yet more generally, in the B model any term which may be written as an integral over the fermionic coordinates does not contribute, whereas in the A-model any term which is an integral over or over does not contribute. This implies that A model observables are independent of the superpotential (as it may be written as an integral over just ) but depend holomorphically on the twisted superpotential, and vice versa for the B model.

Dualities

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Dualities between TSTs

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A number of dualities relate the above theories. The A-model and B-model on two mirror manifolds are related by mirror symmetry, which has been described as a T-duality on a three-torus. The A-model and B-model on the same manifold are conjectured to be related by S-duality, which implies the existence of several new branes, called NS branes by analogy with the NS5-brane, which wrap the same cycles as the original branes but in the opposite theory. Also a combination of the A-model and a sum of the B-model and its conjugate are related to topological M-theory by a kind of dimensional reduction. Here the degrees of freedom of the A-model and the B-models appear to not be simultaneously observable, but rather to have a relation similar to that between position and momentum in quantum mechanics.

The holomorphic anomaly

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The sum of the B-model and its conjugate appears in the above duality because it is the theory whose low energy effective action is expected to be described by Hitchin's formalism. This is because the B-model suffers from a holomorphic anomaly, which states that the dependence on complex quantities, while classically holomorphic, receives nonholomorphic quantum corrections. In Quantum Background Independence in String Theory, Edward Witten argued that this structure is analogous to a structure that one finds geometrically quantizing the space of complex structures. Once this space has been quantized, only half of the dimensions simultaneously commute and so the number of degrees of freedom has been halved. This halving depends on an arbitrary choice, called a polarization. The conjugate model contains the missing degrees of freedom, and so by tensoring the B-model and its conjugate one reobtains all of the missing degrees of freedom and also eliminates the dependence on the arbitrary choice of polarization.

Geometric transitions

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There are also a number of dualities that relate configurations with D-branes, which are described by open strings, to those with branes the branes replaced by flux and with the geometry described by the near-horizon geometry of the lost branes. The latter are described by closed strings.

Perhaps the first such duality is the Gopakumar–Vafa duality, which was introduced by Rajesh Gopakumar and Cumrun Vafa in On the Gauge Theory/Geometry Correspondence. This relates a stack of N D6-branes on a 3-sphere in the A-model on the deformed conifold to the closed string theory of the A-model on a resolved conifold with a B field equal to N times the string coupling constant. The open strings in the A model are described by a U(N) Chern–Simons theory, while the closed string theory on the A-model is described by the Kähler gravity.

Although the conifold is said to be resolved, the area of the blown up two-sphere is zero, it is only the B-field, which is often considered to be the complex part of the area, which is nonvanishing. In fact, as the Chern–Simons theory is topological, one may shrink the volume of the deformed three-sphere to zero and so arrive at the same geometry as in the dual theory.

The mirror dual of this duality is another duality, which relates open strings in the B model on a brane wrapping the 2-cycle in the resolved conifold to closed strings in the B model on the deformed conifold. Open strings in the B-model are described by dimensional reductions of homolomorphic Chern–Simons theory on the branes on which they end, while closed strings in the B model are described by Kodaira–Spencer gravity.

Dualities with other theories

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Crystal melting, quantum foam and U(1) gauge theory

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In the paper Quantum Calabi–Yau and Classical Crystals, Andrei Okounkov, Nicolai Reshetikhin and Cumrun Vafa conjectured that the quantum A-model is dual to a classical melting crystal at a temperature equal to the inverse of the string coupling constant. This conjecture was interpreted in Quantum Foam and Topological Strings, by Amer Iqbal, Nikita Nekrasov, Andrei Okounkov and Cumrun Vafa. They claim that the statistical sum over melting crystal configurations is equivalent to a path integral over changes in spacetime topology supported in small regions with area of order the product of the string coupling constant and α'.

Such configurations, with spacetime full of many small bubbles, dates back to John Archibald Wheeler in 1964, but has rarely appeared in string theory as it is notoriously difficult to make precise. However in this duality the authors are able to cast the dynamics of the quantum foam in the familiar language of a topologically twisted U(1) gauge theory, whose field strength is linearly related to the Kähler form of the A-model. In particular this suggests that the A-model Kähler form should be quantized.

Applications

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A-model topological string theory amplitudes are used to compute prepotentials in N=2 supersymmetric gauge theories in four and five dimensions. The amplitudes of the topological B-model, with fluxes and or branes, are used to compute superpotentials in N=1 supersymmetric gauge theories in four dimensions. Perturbative A model calculations also count BPS states of spinning black holes in five dimensions.

See also

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References

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Revisions and contributorsEdit on WikipediaRead on Wikipedia

Topological string theory

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Topological string theory is a branch of theoretical physics that arises as a topological twist of the worldsheet supersymmetric sigma models in type II superstring theory, resulting in a two-dimensional topological quantum field theory coupled to gravity, designed to compute topological invariants—such as Gromov-Witten invariants and periods—of Calabi-Yau manifolds, which serve as compactification spaces in string theory.[1] Introduced by Edward Witten in 1988, it builds on the N=(2,2) supersymmetry of the underlying sigma models, where the twisting procedure modifies the Lorentz symmetry to produce a topological theory whose correlation functions are independent of the worldsheet metric and depend only on the topology of the target space.[1] This framework simplifies the full dynamics of physical string theory by isolating sectors that capture exact, non-perturbative information about string compactifications on Calabi-Yau threefolds, which are Ricci-flat Kähler manifolds essential for preserving supersymmetry in four-dimensional effective theories.[2] The theory manifests in two primary formulations: the A-model, which relies on the Kähler moduli of the target space and enumerates holomorphic curves through integrals over the moduli space of stable maps, yielding Gromov-Witten invariants that count pseudoholomorphic curves of given genus and degree; and the B-model, which depends on the complex structure moduli and computes integrals of differential forms over the manifold, producing period integrals that encode the geometry's deformations.[2] These models are interconnected via mirror symmetry, a duality conjecture first evidenced in 1991 that equates the A-model on a Calabi-Yau manifold X to the B-model on its mirror manifold X~\tilde{X}, enabling efficient calculations of invariants that would otherwise be computationally intensive—such as the instanton expansion of the prepotential in the quintic Calabi-Yau case.[3] Beyond its mathematical elegance, topological string theory provides crucial insights into physical phenomena, including the exact partition functions of N=2 supersymmetric gauge theories via geometric engineering, the microscopic counting of BPS black hole states in string compactifications, and dualities like the equivalence between Chern-Simons theory on manifolds and A-model invariants on their moduli spaces.[2] Key advancements, such as the holomorphic anomaly equations derived in 1994, allow recursive computation of higher-genus amplitudes FgF_g, bridging perturbative and non-perturbative regimes and influencing broader areas like enumerative algebraic geometry and quantum invariants.[4]

Introduction

Overview

Topological string theory is a topological sector of type II superstring theory, obtained by twisting the N=(2,2) supersymmetric worldsheet theory on Calabi-Yau threefolds as target spaces.[5] In this framework, physical observables become independent of the metric on the target space but depend on either the Kähler or complex structure moduli of the Calabi-Yau manifold. This twisting renders the theory topological, focusing on BRST-invariant quantities that capture global properties rather than local dynamics.[5] The primary motivations for studying topological string theory lie in its simplification of the full superstring theory, allowing computations of topological invariants that are otherwise intractable. It establishes deep connections to enumerative geometry, such as counting holomorphic curves via Gromov-Witten invariants, and to supersymmetric gauge theories, including applications to BPS states and black hole entropy.[5] By isolating these aspects, the theory serves as a powerful toy model to probe broader string theory phenomena. The partition function of topological string theory is given by $ Z = \exp(F) $, where the free energy $ F $ admits a perturbative expansion in the string coupling $ \lambda $:
F=∑gλ2g−2Fg, F = \sum_g \lambda^{2g-2} F_g,
with $ F_g $ denoting the genus-$ g $ contribution.[5] This theory is built from two complementary building blocks: the A-model, which depends on the Kähler moduli and enumerates worldsheet instantons, and the B-model, which relies on the complex structure moduli and involves deformations of holomorphic forms. Mirror symmetry provides a duality that exchanges the A-model on one Calabi-Yau with the B-model on its mirror, linking seemingly distinct geometric structures.

Historical development

The origins of topological string theory trace back to the late 1980s, when Edward Witten introduced topological quantum field theories through the topological twisting of N=2 supersymmetric Yang-Mills theory and sigma models.[6] In his 1988 paper on topological quantum field theory, Witten demonstrated how twisting the Lorentz symmetry with R-symmetry in four-dimensional N=2 supersymmetric Yang-Mills theory yields a topological theory whose observables are Donaldson invariants, establishing a foundational technique for deriving topological invariants from physical models.[6] Extending this approach to two dimensions, Witten's concurrent work on topological sigma models showed that twisting N=2 supersymmetric nonlinear sigma models produces theories independent of the worldsheet metric, with correlation functions computing topological invariants of the target manifold.[7] This twisting mechanism became the cornerstone for subsequent developments in topological string theory. During the early 1990s, topological string theory emerged as a distinct framework, with Witten's 1990 analysis of the topological phase of two-dimensional gravity laying groundwork by relating it to topological minimal models and string-like structures.[8] Cumrun Vafa built on this in 1994 by exploring N=4 topological strings derived from superconformal theories, highlighting their critical dimension and connections to two-dimensional gravity.[9] Concurrently, mirror symmetry was connected to topological strings through the work of Brian Greene and Michael Plesser in the early 1990s, who showed that mirror pairs of Calabi-Yau manifolds exchange the A-model and B-model sectors, providing a duality that equates seemingly different topological invariants. These advances also revealed applications to supersymmetric gauge theories, where topological strings captured non-perturbative effects emerging in the 1990s.[5] Key milestones in the 1990s included the 1993 paper by Mikhail Bershadsky, Stefano Cecotti, Hirosi Ooguri, and Cumrun Vafa, which introduced holomorphic anomaly equations governing the dependence of topological string amplitudes on complex structure moduli, explaining deviations from holomorphy due to worldsheet instantons.[10] Maxim Kontsevich's contributions in the mid-1990s further linked topological strings to enumerative geometry, demonstrating that A-model correlation functions compute Gromov-Witten invariants of symplectic manifolds. In the 2000s, progress accelerated with the introduction of the topological vertex by Mina Aganagic, Albrecht Klemm, Marcos Mariño, and Cumrun Vafa in 2002, a gluing algorithm that computes all-genus amplitudes for toric Calabi-Yau geometries using open string configurations.[11] This tool facilitated large N dualities, such as the equivalence between Chern-Simons theory and open topological strings on the resolved conifold, extending to applications in counting black hole microstates and entropy in string theory.[12] Post-2010 developments focused on non-perturbative definitions, with efforts to incorporate D-brane instantons and resurgence techniques to sum the perturbative series, providing exact partition functions for compact Calabi-Yau manifolds. Refined topological strings, generalizing the unrefined theory by tracking representations of the Heisenberg algebra, saw advances in computational methods, including the refined topological vertex for open amplitudes. Notably, Min-xin Huang and Albrecht Klemm's 2018 work utilized rings of Weyl-invariant Jacobi forms to solve partition functions on elliptic Calabi-Yau threefolds, enabling precise calculations of higher-genus amplitudes and modular properties.[13] Since 2020, further progress has included resurgence analyses of refined topological strings and non-perturbative formulations connecting to spectral theory and 3D BPS indices.[14][15]

Mathematical Foundations

Calabi-Yau manifolds

Calabi-Yau manifolds are compact Kähler manifolds equipped with a Ricci-flat metric, characterized by the vanishing of their first Chern class c1=0c_1 = 0. This condition, proven to admit such metrics by Yau's theorem, ensures the existence of a unique Ricci-flat Kähler metric in each Kähler class. In string theory compactifications, Calabi-Yau manifolds are typically taken to have complex dimension three (Calabi-Yau threefolds), as this dimension allows the ten-dimensional superstring theory to reduce to a four-dimensional theory with N=2\mathcal{N}=2 supersymmetry.[16][17] A defining geometric feature is the presence of a nowhere-vanishing holomorphic (3,0)-form Ω\Omega, which generates the canonical bundle and reflects the manifold's SU(3) holonomy. The topology of these manifolds is captured by Hodge numbers hp,qh^{p,q}, which measure the dimensions of Dolbeault cohomology groups; for threefolds, h1,1h^{1,1} parameterizes the Kähler moduli space, while h2,1h^{2,1} parameterizes the complex structure moduli space. Mirror symmetry, a profound duality in string theory, relates pairs of distinct Calabi-Yau threefolds by interchanging these Hodge numbers, h1,1↔h2,1h^{1,1} \leftrightarrow h^{2,1}, thereby linking invariants computed in different geometric sectors.[18]90559-A)[19] Prominent examples include the quintic hypersurface in CP4\mathbb{CP}^4, defined by the equation ∑i=15zi5=0\sum_{i=1}^5 z_i^5 = 0 with h1,1=1h^{1,1} = 1 and h2,1=101h^{2,1} = 101, serving as a benchmark for enumerative invariants. Toric Calabi-Yau threefolds, constructed via reflexive polyhedra in toric geometry, encompass both compact and non-compact cases, such as the resolved conifold obtained as the total space of O(−1)⊕O(−1)→P1\mathcal{O}(-1) \oplus \mathcal{O}(-1) \to \mathbb{P}^1. K3-fibered Calabi-Yau threefolds, where the base is fibered over a lower-dimensional space with K3 surfaces as fibers, exhibit rich structures exploited in duality studies.[17][20][18] In topological string theory, Calabi-Yau manifolds provide the essential target spaces for the topological A- and B-models, where correlation functions encode cohomological invariants of the manifold. Compactification on these spaces preserves N=2\mathcal{N}=2 supersymmetry in four dimensions, enabling the topological strings to probe geometric features like intersection theory without relying on the full metric details.[18][16]

Special geometry

Special geometry provides the geometric framework for the moduli spaces of Calabi-Yau threefolds in topological string theory, endowing them with a special Kähler structure that governs the low-energy effective action of N=2 supersymmetric theories. The Kähler moduli space is h1,1h^{1,1}-dimensional and parameterized by complexified Kähler parameters ti=Bi+iJit^i = B^i + i J^i, where BiB^i are integrals of the B-field over a basis of H2(X,Z)H_2(X, \mathbb{Z}) and JiJ^i are integrals of the Kähler form JJ over the dual basis of H1,1(X,R)H^{1,1}(X, \mathbb{R}).90321-2) Similarly, the complex structure moduli space is h2,1h^{2,1}-dimensional, parameterized by the periods ΠI=∫γIΩ\Pi^I = \int_{\gamma^I} \Omega of the holomorphic (3,0)(3,0)-form Ω\Omega over a symplectic basis {γI}\{\gamma^I\} of H3(X,Z)H_3(X, \mathbb{Z}). The special Kähler structure on the complex structure moduli space is defined by the Kähler potential
K=−log⁡(i∫XΩ∧Ωˉ), K = -\log \left( i \int_X \Omega \wedge \bar{\Omega} \right),
which induces the Kähler metric gabˉ=∂a∂bˉKg_{a\bar{b}} = \partial_a \partial_{\bar{b}} K. In affine special coordinates ta=Xa/X0t^a = X^a / X^0, where XIX^I are the periods, the geometry is encoded by a holomorphic prepotential F0(t)F_0(t) such that the dual periods are FI=∂F0/∂XIF_I = \partial F_0 / \partial X^I, with the full period vector transforming under the symplectic group Sp(2h2,1+2,Z)Sp(2h^{2,1} + 2, \mathbb{Z}). The Kähler moduli space inherits an analogous structure from the classical prepotential, which at tree level takes the form F0(t)=−16κijktitjtkF_0(t) = -\frac{1}{6} \kappa_{ijk} t^i t^j t^k, where κijk\kappa_{ijk} are the triple intersection numbers.90321-2) Symplectic transformations preserve the special Kähler metric and the pairing ΠTΩΠ\Pi^T \Omega \Pi, where Ω\Omega is the symplectic form, ensuring the consistency of the moduli space geometry across different coordinate patches. The big moduli space extends this framework by incorporating anti-holomorphic deformations, forming a non-compact extension that includes both tt and tˉ\bar{t} directions to accommodate quantum corrections in topological string amplitudes.[21] In the computation of higher-genus topological string amplitudes, non-holomorphic propagators Sab=−14gab+12∂a∂bF(1)S_{ab} = -\frac{1}{4} g_{ab} + \frac{1}{2} \partial_a \partial_b F^{(1)} arise, where F(1)F^{(1)} is the genus-one free energy and gabg_{ab} is the special Kähler metric; these propagators encode the mixing between holomorphic and anti-holomorphic sectors in the big moduli space.[21]

Topological Sigma Models

The A-model

The A-model is a twisted version of the (2,2)(2,2) supersymmetric nonlinear sigma model with a Calabi-Yau manifold as the target space, where the twisting is performed using the vector R-symmetry to promote scalar components of the supercharges to scalars in the twisted theory. This model governs maps from a Riemann surface Σ\Sigma to the target Calabi-Yau threefold XX, emphasizing holomorphic maps in the topological limit. The twisting procedure, which renders the theory topological and independent of the metric on Σ\Sigma, is achieved by identifying the rotation symmetry with part of the Lorentz group, resulting in a BRST symmetry that enforces the topological nature of the correlators.[7] The action of the A-model is given by the path integral ⟨O1⋯On⟩=∫Dϕ Dψ eiS\langle \mathcal{O}_1 \cdots \mathcal{O}_n \rangle = \int \mathcal{D}\phi \, \mathcal{D}\psi \, e^{iS}, where SS is the twisted action including terms such as ∫Σϕi(dϕi+Ai)\int_\Sigma \phi^i (d\phi_i + A_i), with ϕi\phi^i denoting scalar superpartners of the bosonic maps Xi:Σ→XX^i: \Sigma \to X and AA the pullback of a connection on the target. The observables Ok\mathcal{O}_k are BRST-closed operators, typically constructed from cohomology classes on XX, ensuring that the correlators are invariant under deformations of Σ\Sigma. The BRST operator QQ satisfies Q2=0Q^2 = 0 and acts as Q=∫Σ(ψiˉ∂ˉϕi+⋯ )Q = \int_\Sigma (\psi^{\bar{i}} \bar{\partial} \phi_i + \cdots), where ψ\psi are fermionic fields, generating transformations that localize contributions to fixed points of the cohomology operator. This structure makes the theory topological, with correlators computing homotopy invariants of the target.[7] The correlators in the A-model depend solely on the Kähler moduli tit^i of the Calabi-Yau target, parameterized by the complexified Kähler class t=B+iJt = B + iJ, where BB is the B-field and JJ the Kähler form. For genus-gg Riemann surfaces with hh marked points, the correlator ⟨σd1⋯σdh⟩g\langle \sigma_{d_1} \cdots \sigma_{d_h} \rangle_g, where σd\sigma_d inserts a cohomology class Poincaré dual to the homology class of degree dd, equals the Gromov-Witten invariant Nd1,…,dh(g)N_{d_1, \dots, d_h}^{(g)}, which counts the number of stable holomorphic curves of genus gg and degrees did_i in XX, modulo automorphisms. These invariants capture the virtual number of such maps, providing a quantum correction to classical intersection theory on XX.[10] The perturbative expansion of the A-model partition function and correlators is organized in powers of the topological string coupling q=e2πiτq = e^{2\pi i \tau}, where τ\tau is the complex structure on the moduli space of Σ\Sigma. At tree level (g=0g=0), the free energy F0F_0 arises from classical intersection theory on XX, given by triple intersections of divisors in the Kähler cone. Higher-genus contributions FgF_g (g≥1g \geq 1) stem from worldsheet instanton effects, summing over holomorphic maps of all genera, with representative examples including the quintic Calabi-Yau threefold, where the degree-2 instanton number is 609250.[22] This expansion encodes non-perturbative information through the dependence on qs=e−t⋅sq_s = e^{-t \cdot s} for curve classes ss.[10]

The B-model

The B-model is a topological field theory obtained by twisting an N=2 supersymmetric nonlinear sigma model on a Calabi-Yau threefold using the axial U(1)_A R-symmetry, which redefines the Lorentz spins such that the theory becomes independent of the Kähler structure but sensitive to the complex structure of the target space.[23] This twisting promotes two of the supercharges to scalar BRST operators, generating a topological symmetry Q that squares to the Dolbeault operator \bar{\partial}.[23] The resulting theory describes maps from a Riemann surface to the Calabi-Yau target, but the physical content is captured by deformations of the complex structure. The basic fields in the B-model include the bosonic map x:Σ→Xx: \Sigma \to X from the worldsheet Σ\Sigma to the target Calabi-Yau XX, along with fermionic partners: the 1-form ρ\rho (of type (0,1)), the 0-form η\eta (valued in the holomorphic cotangent bundle), and the auxiliary field χ\chi.[17] Central to the model are the Beltrami differentials μ\mu, which are (0,1)-forms on Σ\Sigma valued in the anti-holomorphic tangent bundle of XX, encoding infinitesimal deformations of the complex structure; these serve as the primary observables in the Q-cohomology. The action is fully Q-exact, S=∫ΣQVS = \int_\Sigma Q V, where VV involves terms quadratic in the fields and the Kähler potential, ensuring BRST invariance and metric independence on the worldsheet beyond the moduli.[23] Observables in the B-model are correlation functions of Q-closed operators, corresponding to elements of Hp,qˉ(X,∧rTX)H^{p,\bar{q}}(X, \wedge^r T_X), and are computed as integrals over the moduli space of genus-gg Riemann surfaces with nn marked points: ⟨O1…On⟩g=∫Mg,nev∗(ω1∧⋯∧ωn)\left\langle O_1 \dots O_n \right\rangle_g = \int_{\mathcal{M}_{g,n}} \mathrm{ev}^*(\omega_1 \wedge \dots \wedge \omega_n).[17] Due to the absence of kinetic terms depending on the Kähler metric, the maps degenerate to constant maps, and the correlators factorize into the volume of the moduli space times a factor depending only on the complex structure moduli uau^a via periods of the holomorphic 3-form Ω\Omega over a basis of homology cycles. These periods provide flat coordinates on the moduli space, with the dependence arising from how Ω\Omega varies under complex structure deformations. A fundamental observable is the genus-zero three-point Yukawa coupling Cabc(u)=∫XΩ∧∂a∂b∂cΩC_{abc}(u) = \int_X \Omega \wedge \partial_a \partial_b \partial_c \Omega, where ∂a=∂/∂ua\partial_a = \partial / \partial u^a acts on the moduli-dependent Ω\Omega, capturing the cubic interactions in the effective theory.[17] The tree-level prepotential F0(u)F_0(u) is constructed from these periods as F0=12XIFI+16κIJKXIXJXKF_0 = \frac{1}{2} X^I F_I + \frac{1}{6} \kappa_{IJK} X^I X^J X^K, where XI=∫AIΩX^I = \int_{A_I} \Omega and FI=∫BIΩF_I = \int_{B^I} \Omega over dual symplectic cycles, with κIJK\kappa_{IJK} the intersection numbers; higher-genus amplitudes deform this prepotential via quantum corrections to the periods.[17] The Yukawa couplings are the third derivatives Cabc=∂a∂b∂cF0C_{abc} = \partial_a \partial_b \partial_c F_0.[17] The B-model correlators encode the deformation theory of the complex structure, with the Beltrami differentials generating the Kodaira-Spencer dg-Lie algebra whose cohomology controls infinitesimal deformations in H1(X,TX)H^1(X, T_X). Higher-point functions compute obstructions to lifting these deformations to higher orders, residing in H2(X,TX)H^2(X, T_X), while multi-genus correlators yield higher cohomology operations and Massey products in the deformation complex.[23] Under mirror symmetry, the B-model on XX is dual to the A-model on the mirror Calabi-Yau X~\tilde{X}, exchanging complex and Kähler structures.[17]

Topological twisting

Topological twisting transforms the N=2 supersymmetric sigma model into a topological quantum field theory by redefining the spins of the worldsheet fields using the R-symmetry currents. In the A-model, the Lorentz spin $ s' $ is modified as $ s' = s + \frac{1}{2} F_V $, where $ F_V $ is the vector R-symmetry generator, while in the B-model, it is $ s' = s + \frac{1}{2} F_A $, with $ F_A $ the axial R-symmetry generator. This adjustment promotes one of the supercharges to a scalar under the new Lorentz group, enabling the identification of a BRST operator $ Q $ that squares to zero and renders the action $ Q $-exact up to a topological term.[24] The BRST operator $ Q $ in these twisted theories takes the form $ Q = \int (c \bar{\partial} + \psi^i \nabla_i + \cdots) $, where $ c $ is the reparametrization ghost, $ \psi^i $ are the fermionic partners, and the ellipsis denotes additional terms involving auxiliary fields and connections on the target space; its nilpotency $ Q^2 = 0 $ holds up to gauge transformations or equations of motion. This structure ensures that physical observables, defined as $ Q $-closed operators, lie in the cohomology of $ Q $, making the theory independent of continuous deformations of the worldsheet metric.[25][24] Invariance under worldsheet metric variations arises because the path integral localizes to fixed-point contributions: in the A-model, to holomorphic maps from the worldsheet to the target Calabi-Yau manifold, and in the B-model, to constant maps. Consequently, correlation functions of $ Q $-closed operators are metric-independent and capture topological invariants of the target space.[24] The correlators in these theories compute elements of the cohomology groups of the target manifold, yielding invariants analogous to those in Donaldson-Witten theory for gauge configurations or in superconformal field theories. For instance, on a toroidal worldsheet, the partition function relates to the elliptic genus, providing a measure of the SCFT's topological properties.[24] This twisting mechanism applies to both A- and B-models and extends to topological string theory through the inclusion of dynamical gravity in the twisted sector.[24]

Topological Strings

Partition function and observables

In topological string theory, the partition function ZZ encodes the perturbative expansion in the string coupling constant λ\lambda, given by
Z=exp⁡(∑g=0∞λ2g−2Fg), Z = \exp\left( \sum_{g=0}^\infty \lambda^{2g-2} F_g \right),
where FgF_g denotes the genus-gg free energy or amplitude. Each FgF_g arises from an integral over the moduli space Mg,n\mathcal{M}_{g,n} of genus-gg Riemann surfaces with nn marked points,
Fg=∫Mg,nω(β1)∧⋯∧ω(βn), F_g = \int_{\mathcal{M}_{g,n}} \omega(\beta_1) \wedge \cdots \wedge \omega(\beta_n),
with ω(βi)\omega(\beta_i) representing the descent forms associated to cohomology classes βi∈H∗(X)\beta_i \in H^*(X), and σβi\sigma_{\beta_i} the corresponding chiral primary operators in the twisted N=2N=2 superconformal field theory on the worldsheet. These descent forms ensure that the correlators are metric-independent and localize to topological invariants, such as intersections in the target Calabi-Yau manifold XX.[10] The observables in topological string theory are captured by multi-point correlators ⟨σβ1⋯σβn⟩g\langle \sigma_{\beta_1} \cdots \sigma_{\beta_n} \rangle_g at genus gg, which physically interpret as weighted counts of BPS states bound to the worldsheet.[5] In the A-model, these depend solely on the Kähler moduli tit^i, complexified volumes of two-cycles in XX, reflecting contributions from worldsheet instantons wrapping holomorphic curves. Conversely, in the B-model, the dependence is on the complex structure moduli uau^a, parameterized by periods of the holomorphic three-form over homology cycles, and arises from deformations in the Dolbeault cohomology of XX. This metric independence underscores the topological nature, with the BPS interpretation linking the correlators to protected sectors of the full string theory spectrum, such as half-BPS states in four-dimensional N=2\mathcal{N}=2 supersymmetric theories.[5] The genus expansion begins with the classical term F0F_0, which for the A-model includes the triple intersection of the Kähler form plus a worldsheet instanton sum, while for the B-model it is the classical prepotential 12XIFI\frac{1}{2} X_I F^I expressed in terms of periods.[5] At one-loop, F1F_1 provides quantum corrections; in the A-model, it takes the form F1=−log⁡det⁡+112c2⋅tF_1 = -\log \det + \frac{1}{12} c_2 \cdot t, where det⁡\det involves the determinant over the moduli space and c2⋅tc_2 \cdot t is the contraction of the second Chern class with the Kähler parameters.[10] Higher-genus terms FgF_g (for g≥2g \geq 2) receive non-holomorphic corrections via the holomorphic anomaly, ensuring consistency with S-duality, though the perturbative objects remain formally holomorphic in the moduli.[10] These amplitudes play a central role in dualities, such as mirror symmetry, where A-model invariants on one Calabi-Yau map to B-model periods on the mirror.[5]

Holomorphic anomaly equations

The holomorphic anomaly equations (HAE) govern the dependence of the topological string free energies FgF_g on the anti-holomorphic moduli tˉk\bar{t}^k, arising from an anomaly in the conformal symmetry of the underlying N=2N=2 superconformal field theory coupled to topological gravity.[10] This anomaly manifests as a failure of BRST-trivial states to decouple completely, leading to mixing between holomorphic and anti-holomorphic sectors in the correlation functions.[10] Introduced by Bershadsky, Cecotti, Ooguri, and Vafa in their 1993 paper, the HAE provide recursive partial differential equations that determine the higher-genus amplitudes FgF_g (for g≥1g \geq 1) up to holomorphic ambiguities fixed by boundary conditions.[10] The central equation for the genus-gg free energy, with g≥2g \geq 2, takes the form
∂ˉıˉFg=12∑j,kCjklCˉıˉjˉkˉ   lˉ(DjDkFg−1+∑r=1g−1DjFr DkFg−r), \bar{\partial}_{\bar{\imath}} F_g = \frac{1}{2} \sum_{j,k} C_{j k l} \bar{C}_{\bar{\imath} \bar{j} \bar{k}}^{\ \ \ \bar{l}} \left( D^j D^k F_{g-1} + \sum_{r=1}^{g-1} D^j F_r \, D^k F_{g-r} \right),
where ∂ˉıˉ\bar{\partial}_{\bar{\imath}} denotes the anti-holomorphic derivative with respect to tˉıˉ\bar{t}^{\bar{\imath}}, CjklC_{jkl} are the triple intersection numbers on the Calabi-Yau threefold (encoding the classical Yukawa couplings in the B-model), Cˉ\bar{C} are the complex conjugates, and DiD^i are covariant derivatives with respect to the Kähler connection on the moduli space of special geometry (the full expression includes factors like e2KGlˉme^{2K} G^{\bar{l} m} from the metric and Kähler potential).[10] The indices run over the complex structure or Kähler moduli, depending on the topological string model. For genus one (g=1g=1), a similar but modified equation holds, involving the Weil-Petersson metric and the Euler characteristic χ\chi of the Calabi-Yau.[10] The free energies Fg(t,tˉ)F_g(t, \bar{t}) are holomorphic in the moduli tit^i but acquire anti-holomorphic dependence tˉjˉ\bar{t}^{\bar{j}} through the anomaly, reflecting the non-topological aspects of the underlying sigma model.[10] This structure allows a recursive solution: starting from the classical F0F_0 (the prepotential) and the genus-one F1F_1, higher FgF_g are built iteratively using non-holomorphic propagators SijS_{ij}, defined via the genus-one anomaly equation, along with boundary conditions in the topological limit tˉ→i∞\bar{t} \to i \infty, where the anti-holomorphic dependence decouples and FgF_g reduces to a holomorphic function counting BPS invariants. [26] A representative example is the one-parameter quintic Calabi-Yau threefold, where the genus-one free energy in the large volume limit includes the term
F1=5012t+⋯ , F_1 = \frac{50}{12} t + \cdots,
with tt the Kähler parameter (related to the integral of the Kähler form over the hyperplane class, incorporating the universal ∫c2⋅t/12\int c_2 \cdot t / 12 term from the second Chern class c2c_2, where c2⋅H=50c_2 \cdot H = 50); on the mirror quintic, the B-model expansion in the large complex structure limit captures quantum corrections including ζ(3)\zeta(3) terms via the periods.[10] [3] For higher genera, the solutions take the form of polynomials in the propagators SijS_{ij}, such as Fg=∑Pg,ij(F0,…,Fg−1)SijF_g = \sum P_{g,ij}(F_0, \dots, F_{g-1}) S^{ij} for the leading terms, leveraging the ring structure generated by the anomaly.[26] The HAE imply a non-perturbative ambiguity in the holomorphic topological limit, arising from undetermined holomorphic functions that encode worldsheet instanton and D-brane effects beyond perturbation theory.[27] Direct integration techniques, which solve the equations by expressing FgF_g in terms of explicit integrals over the moduli space, have been developed to resolve these ambiguities for specific geometries, as demonstrated in the 2007 work of Grimm, Klemm, Mariño, and Weiss.[27]

Dualities and Relations

Mirror symmetry

Mirror symmetry in topological string theory establishes a profound duality between the A-model and the B-model defined on a pair of mirror Calabi-Yau threefolds XX and X^\hat{X}. The A-model, which depends on the Kähler moduli tit^i of XX, computes observables such as Gromov-Witten invariants through worldsheet instantons. In contrast, the B-model relies on the complex structure moduli uau^a of X^\hat{X} and involves period integrals of the holomorphic three-form. This duality exchanges the roles of these moduli spaces, with the mirror map providing a coordinate transformation that identifies flat coordinates on one side with those on the other, ensuring that physical quantities match across the duality.[28] The key statement of mirror symmetry relates the genus-gg free energies FgF_g of the topological string partition function. Specifically, under the mirror map u^(t)\hat{u}(t) that exchanges Kähler moduli tit^i of XX with complex moduli uau^a of X^\hat{X}, the relation holds:
Fg(t)=(−1)gFg(u^(t)) F_g(t) = (-1)^g F_g(\hat{u}(t))

for the B-model periods, where the sign alternation arises from the orientation conventions in the A- and B-model path integrals. This equality implies that instanton corrections in the A-model correspond to perturbative expansions around the large complex structure point in the B-model. Mirror symmetry also exchanges the Hodge numbers of the Calabi-Yau manifolds, with h1,1(X)=h2,1(X^)h^{1,1}(X) = h^{2,1}(\hat{X}) and h2,1(X)=h1,1(X^)h^{2,1}(X) = h^{1,1}(\hat{X}).[28] A canonical example is the mirror pair involving the quintic Calabi-Yau hypersurface in P4\mathbb{P}^4, defined by a degree-5 polynomial, and its mirror constructed as an orbifold quotient with parameter ψ5\psi^5. Here, the A-model on the quintic yields rational curve counts via the instanton expansion Finst(q)=∑d>0ndqdF_\text{inst}(q) = \sum_{d>0} n_d q^d, where q=e2πitq = e^{2\pi i t} and ndn_d are the degrees of rational curves. The mirror map aligns this with B-model periods solving the Picard-Fuchs equation [θ4−5z(5θ+4)(5θ+3)(5θ+2)(5θ+1)]Π=0[\theta^4 - 5z (5\theta + 4)(5\theta + 3)(5\theta + 2)(5\theta + 1)] \Pi = 0, where θ=zddz\theta = z \frac{d}{dz} is the logarithmic derivative and Π\Pi denotes the period vector. The Gauss-Manin connection LL governs the variation of these periods, satisfying ∇LΠ=0\nabla_L \Pi = 0, which encodes the monodromy around the discriminant locus. Computations confirm that the instanton numbers ndn_d match the series expansion of the periods near the conifold point.[29][28] For toric Calabi-Yau manifolds, mirror symmetry manifests through dual descriptions involving spectral curves. In these cases, the mirror to a toric variety is often a Landau-Ginzburg model or a resolved conifold geometry, where the spectral curve arises as the Riemann surface defining the B-model periods. The mirror map equates Kähler parameters of the toric phase with complex structure parameters of the mirror, allowing instanton expansions in the A-model to be matched against recursive solutions of Picard-Fuchs equations on the spectral curve. This framework facilitates explicit computations for geometries like O(−3)⊕O(−3)→P2\mathcal{O}(-3) \oplus \mathcal{O}(-3) \to \mathbb{P}^2.[28][30] An important extension is homological mirror symmetry, proposed by Kontsevich, which conjectures an equivalence between the derived category of coherent sheaves on XX (relevant to the B-model) and the Fukaya category of Lagrangian submanifolds in the symplectic manifold X^\hat{X} (relevant to the A-model). This categorical duality underpins the exchange of D-brane categories across the mirror and provides a homological algebra framework for understanding non-perturbative aspects of topological strings.[31][28]

Geometric transitions

Geometric transitions in topological string theory describe dualities that alter the topology of the target Calabi-Yau threefold, relating geometries with resolved singularities to those with deformations while preserving the string partition function and observables. These transitions involve shrinking exceptional cycles, such as P1≅S2\mathbb{P}^1 \cong S^2 in a resolved configuration, and replacing them with deformed cycles, like S3S^3, accompanied by the creation of fluxes that stabilize the new geometry. This process connects open topological string amplitudes, computed with branes wrapping the resolved cycles, to closed string amplitudes on the deformed background. A canonical example is the conifold transition, where the resolved conifold—obtained by blowing up the singular point of the quintic hypersurface equation xy−uv=ϵxy - uv = \epsilon with ϵ>0\epsilon > 0, introducing a P1\mathbb{P}^1—transitions to the deformed conifold defined by xy−uv=μxy - uv = \mu with μ≠0\mu \neq 0, featuring an S3S^3 of radius proportional to ∣μ∣1/2|\mu|^{1/2}. In this duality, the open A-model on the resolved conifold, involving D-branes on the P1\mathbb{P}^1, is equivalent to the closed topological string on the deformed conifold. The transition is interpreted as a large NN duality akin to AdS/CFT, where NN branes on the resolved side yield a gauge theory whose planar limit matches the closed string genus expansion on the deformed side.[32] The partition functions across the transition exhibit precise matching. On the resolved conifold, the A-model partition function, encoding higher-genus free energies FgF_g, is computed via the topological vertex formalism, which glues together cubic vertices to sum over worldsheet instantons wrapping toric legs.[11] On the deformed conifold, the dual B-model partition function arises from integrating over the periods of the deformed geometry, capturing the same non-perturbative structure without branes. In the matrix model description of the duality, the radius of the S3S^3 corresponds to the cut in the eigenvalue distribution, reflecting the volume-filling transition at large NN.[32][5] Vafa's construction establishes that geometric transitions generate broader dualities between open and closed topological string formulations, embedding them within superstring theory and ensuring consistency of observables like the holomorphic anomaly equations across the transition.[12] Mirror symmetry relates the A- and B-models on each side of the transition independently.[32]

Connections to gauge theories and M-theory

Topological string theory exhibits profound dualities with supersymmetric gauge theories, particularly through brane configurations in type IIA string theory. In the large NN limit, the partition function of N=2\mathcal{N}=2 SU(NN) supersymmetric gauge theory on R4\mathbb{R}^4 with adjoint hypermultiplets matches the topological A-model partition function on a toric Calabi-Yau threefold, realized via stacks of NN D-branes wrapping the toric geometry. This duality arises from the open-closed string correspondence, where open string states on the D-branes encode gauge theory dynamics, transitioning to closed topological strings in the large NN regime.[33] Additionally, the Seiberg-Witten curve governing the low-energy effective theory of N=2\mathcal{N}=2 SU(2) gauge theory emerges as the mirror Riemann surface to the type IIA brane setup on a local Calabi-Yau, providing a geometric interpretation of the gauge theory moduli space. A key computational tool in this framework is the topological vertex, a combinatorial formalism that generates all-genus amplitudes of the topological A-model on non-compact toric Calabi-Yau threefolds by summing over configurations of D-branes at toric fixed points.[11] This vertex glues together to form the full A-model partition function via a cut-and-paste procedure along the toric diagram edges, effectively capturing the contributions from brane intersections and relating them to open string invariants.[34] The topological vertex further connects to statistical models of crystal melting, where the melting process of a three-dimensional crystal dual to the toric geometry counts BPS bound states of D0- and D2-branes on a D6-brane probe, mirroring the gauge theory Higgs branch. In the M-theory uplift, topological string theory on Calabi-Yau threefolds lifts to topological M-theory in 11 dimensions, where the type IIA topological strings emerge as a dimensional reduction.[35] Here, the Gopakumar-Vafa invariants, which refine the genus expansion of the topological string partition function into integer BPS counts, arise from M2-branes wrapping supersymmetric three-cycles in the resolved Calabi-Yau geometry, providing a non-perturbative definition independent of the perturbative series. Non-perturbative effects in topological strings, such as those from worldsheet instantons, find an interpretation as quantum foam in the presence of a U(1) gauge theory realized by a single D6-brane wrapping the Calabi-Yau.[36] These effects manifest as fluctuating configurations of the D6-brane, akin to a foamy geometry at the string scale, with the average shape governed by the topological string free energy; crystal melting models describe the Higgs branch vacua of this setup, linking to the non-perturbative BPS spectrum.[36]

Applications

Enumerative invariants

In topological A-model string theory, the correlators compute Gromov-Witten invariants, which enumerate the number of stable holomorphic maps from genus-gg Riemann surfaces with nn marked points to a Calabi-Yau threefold XX, modulo automorphisms of the domain. These invariants, denoted Ng,n(β)N_{g,n}(\beta) for curve class β∈H2(X,Z)\beta \in H_2(X,\mathbb{Z}), are given by
Ng,n(β)=1∣Aut(C)∣⟨∏i=1nevi∗γji⟩g,n,β, N_{g,n}(\beta) = \frac{1}{|\mathrm{Aut}(\mathcal{C})|} \left\langle \prod_{i=1}^n \mathrm{ev}_i^* \gamma_{j_i} \right\rangle_{g,n,\beta},
where evi\mathrm{ev}_i are evaluation maps at marked points, γji\gamma_{j_i} are cohomology classes on XX, and the correlator is the A-model expectation value in the sector of degree β\beta. The partition function of the A-model encodes these invariants through its genus and multi-point expansion. Refined Gromov-Witten invariants extend these counts by incorporating additional structure via refinement parameters qq and tt, which track Hodge-theoretic data such as the Hodge polynomial of the moduli space of curves, providing refined BPS state counts. In the context of topological strings, these refined invariants arise from the refined topological vertex formalism, capturing contributions from both bosonic and fermionic degrees of freedom in BPS sectors.[37] Donaldson-Thomas invariants, which count invariant subschemes of ideal sheaves on XX with fixed Chern character, are computed in the B-model via the partition function's plethystic expansion or non-compact limits, often leveraging mirror symmetry for explicit evaluation.[38] A prominent example is the genus-zero Gromov-Witten invariant of the quintic Calabi-Yau threefold in P4\mathbb{P}^4, where the number of rational curves of degree 1 through 3 generic points is n0,1,1=2875n_{0,1,1} = 2875, a classical enumerative geometry result confirmed by mirror symmetry in the topological string framework.[3] Higher-genus invariants for the quintic are obtained by solving the holomorphic anomaly equations, which recursively determine the genus-gg contributions from lower-genus data and boundary terms. For toric Calabi-Yau threefolds, the topological vertex provides an explicit combinatorial formula for all-genus Gromov-Witten invariants as sums over Young tableaux glued along edges, representing open string contributions from branes on toric boundaries. A simple case is the local CP1\mathbb{CP}^1 geometry, equivalent to the resolved conifold, where the vertex yields the generating function ∑gNgqg=q1/2(q;q)∞(q−1;q)∞\sum_g N_g q^g = \frac{q^{1/2}}{(q;q)_\infty (q^{-1};q)_\infty} for the invariants NgN_g in the zero-degree sector, with N0=1N_0 = 1.

Supersymmetric gauge theories

Topological string theory offers powerful tools for deriving exact results in supersymmetric gauge theories, particularly by realizing their dynamics through dual geometric configurations on Calabi-Yau manifolds. In the context of N=2 theories, these dualities map perturbative and non-perturbative effects, such as instantons and monopoles, to topological invariants computable via string amplitudes. This framework not only reproduces classical solutions like the Seiberg-Witten effective theory but also extends to higher-dimensional N=1 setups, providing insights into vacuum structures and partition functions. A key application is the large N duality between the topological B-model on a deformed Calabi-Yau threefold and softly broken N=2 SU(N) gauge theories. Proposed by Dijkgraaf and Vafa, this duality equates the planar limit of a one-cut matrix model—encoding the glueball superpotential of the N=2* theory deformed by a tree-level superpotential for the adjoint chiral multiplet—to the B-model amplitudes on the local deformed geometry. In the large N limit, the effective dynamics of the gauge theory, including non-perturbative effects from gaugino condensation, are captured by the topological string free energy. The prepotential of the unbroken N=2 theory emerges from the special geometry of the periods on the deformed Calabi-Yau, with higher-genus corrections corresponding to worldsheet instantons in the B-model. This connection, realized via geometric transitions from resolved to deformed geometries, allows exact computation of the gauge theory's F-terms beyond perturbation theory.[33] The Seiberg-Witten curve, central to the exact solution of N=2 supersymmetric Yang-Mills theories, finds a natural interpretation in topological string theory through mirror symmetry. For pure SU(2) or more general gauge groups, the curve—a hyperelliptic Riemann surface encoding the Coulomb branch and BPS spectrum—is the mirror dual to the resolved local Calabi-Yau geometry associated with the ultraviolet completion of the gauge theory. In this duality, electric and magnetic charges correspond to cycles on the resolved side, while the deformed mirror encodes the infrared dynamics. Magnetic monopoles, which become massless at strong coupling points and drive the quantum moduli space, are realized as D-branes wrapping non-compact cycles in the type IIA string embedding of the theory; specifically, they arise as bound states of D4-branes ending on NS5-branes in the brane configuration, lifting to M2-branes in M-theory on the Calabi-Yau times a circle. This brane picture not only reproduces the dyon spectrum but also aligns the topological A-model invariants on the resolved geometry with the Seiberg-Witten periods, confirming the non-perturbative duality structure. Refined topological strings further bridge to the instanton calculus of N=2 gauge theories via the Nekrasov partition function. The refinement introduces two topological twisting parameters, refining the BPS counting and matching the equivariant Donaldson-Thomas invariants on the resolved Calabi-Yau to the Nekrasov sum over Yang-Mills instantons weighted by fugacities for the Cartan torus action. For SU(N) theories with matter, the refined topological string free energy on toric geometries computes the exact prepotential, including all orders in the instanton expansion, as the logarithm of the Nekrasov partition function in the omega-background. This equivalence, established through the refined topological vertex formalism, provides a geometric resummation of the perturbative gauge theory series and extends the Seiberg-Witten solution to include refined BPS indices. In five-dimensional N=1 supersymmetric gauge theories engineered by D-branes probing toric Calabi-Yau threefolds, topological strings describe the vacuum structure via crystal melting models. These theories, obtained by compactification of M-theory on the toric geometry, feature Coulomb branches parameterized by vevs of vector multiplets, with vacua corresponding to resolved phases of the geometry. The crystal melting picture, developed by Okuyama and Sakai, models BPS bound states of D0- and D2-branes on a D6-brane wrapping the toric Calabi-Yau as a statistical ensemble of melting 3D crystals, where each melting configuration represents a Higgs vacuum of the gauge theory. The partition function of the melting crystal, governed by the topological string amplitudes on the resolved toric manifold, counts these vacua and reproduces the Nekrasov-like instanton sums for 5D theories, including Kaluza-Klein modes from the extra dimension. This approach highlights the melting cycles as geometric analogs of the gauge theory's moduli, with phase transitions mirroring wall-crossing in the BPS spectrum.[39]

Black hole entropy

In type IIA string theory compactified on a Calabi-Yau threefold, four-dimensional BPS black holes can be realized as bound states of D0-, D2-, D4-, and D6-branes wrapping cycles of the Calabi-Yau manifold. The macroscopic Bekenstein-Hawking entropy of these extremal black holes is given by $ S = 2\pi \sqrt{|Z|} $, where $ Z $ is the central charge determined by the attractor mechanism at the black hole horizon. Microscopically, this entropy is reproduced by the partition function of the topological A-model string on the resolved Calabi-Yau geometry, which counts BPS invariants associated with the brane configurations; the logarithm of this partition function, evaluated at the attractor point in moduli space, matches the entropy function up to subleading corrections. The topological string free energy encodes these BPS states through Gopakumar-Vafa invariants, which refine the rational Gromov-Witten invariants into integer-valued BPS indices $ n_{g,k} $ that count bound states of multi-wrapped curves with spin contributions. The genus-$ g $ free energy term $ F_g $ is expressed as a series involving these invariants, $ F_g = \sum_{k \geq 1} \sum_d n_{g,k}(d) \frac{(-1)^{kg}}{k^{2g-2}} \mathrm{Li}_{2g-2}(q^{kd}) $, where $ q = e^{2\pi i \tau} $ and $ \mathrm{Li} $ denotes the polylogarithm; this structure arises from S-duality invariance, ensuring the invariants' rationality and integrality. These invariants provide a non-perturbative definition of the topological string partition function, directly linking enumerative geometry to the black hole microstate degeneracy. In five dimensions, BPS black holes arise from M-theory compactified on a Calabi-Yau threefold, described by M2- and M5-brane wrappings that reduce to D-brane systems upon further compactification. The microscopic entropy is computed via the partition function of topological strings on the Calabi-Yau, interpreted through topological M-strings whose worldsheet theory captures the BPS spectrum; this yields the exact degeneracy matching the macroscopic area law. The Ooguri-Strominger-Vafa (OSV) conjecture extends non-perturbatively to five dimensions, proposing that the refined topological string free energy generates the BPS indices for these black holes, incorporating higher-genus contributions beyond weak-coupling limits. A seminal example is the Strominger-Vafa black hole in five dimensions, constructed from M2-branes wrapping curves in the Calabi-Yau and carrying large charges; the topological string partition function $ Z_{\mathrm{top}} $ satisfies $ \log |Z_{\mathrm{top}}| \approx S/2 $ in the Cardy regime of high temperature, reproducing the exact Bekenstein-Hawking entropy $ S = 2\pi \sqrt{n_1 n_5 Q_1 Q_5 / 6} $ from the microscopic count of BPS states.[40] This match validates the duality between the weakly coupled brane microstates and the strongly coupled supergravity solution, with logarithmic corrections aligning via the topological string's holomorphic anomaly.

References

  1. https://doi.org/10.1007/BF02100054
  2. [PDF] A mini-course on topological strings - arXiv
  3. https://doi.org/10.1016/0550-3213(91
  4. https://doi.org/10.1007/BF02099559
  5. [hep-th/0410178] Topological strings and their physical applications
  6. Topological quantum field theory | Communications in Mathematical ...
  7. Topological sigma models | Communications in Mathematical Physics
  8. On the structure of the topological phase of two-dimensional gravity
  9. N=4 topological strings - Inspire HEP
  10. Holomorphic Anomalies in Topological Field Theories - arXiv
  11. [hep-th/0305132] The Topological Vertex - arXiv
  12. [hep-th/0008142] Superstrings and Topological Strings at Large N
  13. [1712.07017] Topological Strings on Singular Elliptic Calabi-Yau 3 ...
  14. https://doi.org/10.1016/0550-3213(85
  15. [PDF] An introduction to topological string theory
  16. [PDF] Introduction in Topological String Theory on Calabi-Yau manifolds
  17. https://doi.org/10.1007/BF02100731
  18. https://doi.org/10.1016/0550-3213(93
  19. The topological sigma model
  20. [hep-th/9112056] Mirror Manifolds And Topological Field Theory
  21. Physics The Topological Sigma Model - Project Euclid
  22. BCOV ring and holomorphic anomaly equation - Project Euclid
  23. [hep-th/0702187] Direct Integration of the Topological String - arXiv
  24. [PDF] Mirror Symmetry | Clay Mathematics Institute
  25. AMS :: Journal of the American Mathematical Society
  26. [1506.07757] Spectral Theory and Mirror Symmetry - arXiv
  27. [alg-geom/9411018] Homological Algebra of Mirror Symmetry - arXiv
  28. [hep-th/0103067] A Large N Duality via a Geometric Transition - arXiv
  29. [hep-th/0206255] Matrix Models, Topological Strings, and ... - arXiv
  30. The Topological Vertex | Communications in Mathematical Physics
  31. [hep-th/9812127] M-Theory and Topological Strings--II - arXiv
  32. [hep-th/0312022] Quantum Foam and Topological Strings - arXiv
  33. [hep-th/0410018] Topological String Amplitudes, Complete ... - arXiv
  34. [0811.2801] Crystal Melting and Toric Calabi-Yau Manifolds - arXiv
  35. Microscopic Origin of the Bekenstein-Hawking Entropy - hep-th - arXiv
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