New Supersymmetric Localizations from Topological Gravity

Supersymmetric field theories can be studied exactly on suitable off-shell supergravity backgrounds. We show that in two dimensions such backgrounds are identifiable with BRST invariant backgrounds of topological gravity coupled to an abelian topological gauge multiplet. This latter background is required for the consistent coupling of the topological `matter' YM theory to topological gravity. We make use of this topological point of view to obtain, in a simple and straightforward way, a complete classification of localizing supersymmetric backgrounds in two dimensions. The BRST invariant topological backgrounds are parametrized by both Killing vectors and $S^1$-equivariant cohomology of the 2-dimensional world-sheet. We reconstruct completely the supergravity backgrounds from the topological data: some of the supergravity fields are twisted versions of the topological backgrounds, but others are"composite", i.e. they are non-linear functionals of them. We recover all the known localizing 2-dimensional backgrounds and (infinitely) many more that have not been explored so far. We show that the supersymmetric $\Omega$-deformation is nothing but the background value of the ghost-for-ghost of topological gravity, a result which holds for other dimensions too. The new localizing backgrounds are characterized by non-trivial fluxes for both the graviphotons of the supergravity multiplet.


Introduction and Summary
The localization technique refers to an exact WKB method by virtue of which the semiclassical approximation becomes exact. It has been extensively studied for a broad class of quantum field theories that admit Lagrangian descriptions, in particular, supersymmetric or topological quantum field theories. For instance, the topological quantum field theories (TQFTs) whose action is BRST-exact 1 are semi-classically exact since their coupling constant is a gauge parameter which can be taken arbitrarily small. A traditional route for constructing TQFTs is by topologically twisting supersymmetric quantum field theories (SQFTs) by means of a conserved R-symmetry. Hence, the localization technique has frequently been associated to SQFTs since the early days.
Recently, starting from the work [1], localization technique has been revived for various SQFTs, without connecting it to TQFTs in any explicit manner. Rather, in this point of view, localization is the consequence of the existence of a global (nilpotent on physical states) supercharge when the SQFT is defined on specific external backgrounds. These external backgrounds may be identified, as done first in [2], with an off-shell configuration of a supergravity (SG) multiplet that the SQFT can couple to. Global supercharges of the SQFT are in correspondence with generalized covariantly constant spinors that set the supersymmetry variations of fermionic fields of the SG multiplet to zero.
The generalized covariantly constant spinor must satisfy integrability conditions which put stringent constraints on the bosonic fields of the SG multiplet. These fields include the spacetime metric and also, in theories with extended supersymmetries, vector fields of gauged R-symmetries as well as off-shell auxiliary fields. It turns out that, in general, the bosonic fields of the SG multiplet must be switched on for the SQFT to be put supersymmetrically on a -compact or noncompact -curved manifold supporting generalized covariantly constant spinors. The background bosonic fields are external sources for associated conserved current operators of the SQFT, thus parametrize the space of deformed SQFT. Hereafter, we shall refer to this space of SQFTs as the matter SQFT.
Generalized covariantly constant spinors depend on the spacetime dimensions and also on the specific SG to which the matter SQFT is coupled. The localization technique to matter SQFT is applicable when the space of generalized covariantly constant spinors is nonempty. A complete classification of generalized covariantly constant spinors is a complicated problem. Although explicit solutions have been obtained case by case in various spacetime dimensions, there is no general strategy for constructing the covariantly constant spinors and for classifying the background spacetime metrics and gauge fields which support them.
In this paper, we put forward a new approach for finding localizing backgrounds for matter SQFTs. The strategy of our approach -which was already introduced by two of the authors of the present paper in the context of three-dimensional N = 2 supersymmetric gauge theories [3] -is the following: one starts from a SQFT and twists it to obtain a corresponding topological matter theory which is then coupled to topological gravity (TG) backgrounds. One then seeks for BRST-invariant backgrounds: each BRST-invariant background is associated with a topological matter theory. The trivial background, of course, corresponds to the original topological matter theory. Non-trivial topological backgrounds define new topological matter theories whose deformations are associated to the geometrical structures parametrizing the BRST-invariant backgrounds.
In the present paper, we apply this topological approach to two-dimensional matter SQFT and we elaborate on its general features. We will see that the equations for covariantly constant spinors of two-dimensional N = (2, 2) supergravity are recast in the topological framework as cohomological equations. Specifically, we show that the generalized covariantly constant spinors are expressed in terms of S 1 -equivariant de Rham cohomology of the underlying spacetime. The cohomological formulation incorporates automatically the concept of gauge equivalent topological gravity backgrounds. We work out the explicit map between the BRST invariant topological backgrounds and the supersymmetry-preserving two-dimensional N = (2, 2) supergravity backgrounds: this map allows therefore to identify supergravity backgrounds which are equivalent for localization purposes. To the best of our knowledge, the concept of equivalent generalized covariantly constant spinors is new and appears to be one major benefit of our approach. We also explicitly construct all the inequivalent localizing SG backgrounds. We recover the solutions found in previous works [4] - [7] and also many more new ones: in fact, infinitely many more.
The equations for the BRST invariant topological backgrounds are the topological counterpart of the equations for the generalized covariantly constant spinors of SG. However, contrary to the naïve expectation, the topological gravity system which is relevant in our framework is not a topological twist of the supergravity of the standard approach. In fact, the relation that we uncover between the generalized covariantly constant spinors of the supergravity approach and the solutions of the cohomological equations of the topological approach is non-trivial. Most of topological bosonic background fields are not, in any sense, bosonic fields of topologically twisted SG. Several of the BRST invariant topological back-grounds are bilinears of the covariantly constant spinors of supergravity. For example, the ghost-for-ghost field 2 of TG is identified with the spinorial bilinear which defines the Killing vector of the spacetime metric. Conversely, the SG fields which correspond to a BRST invariant topological background are, in general, non-linear functionals of the fields of TG. In this work, we explicitly construct these functionals for the specific case of two-dimensional N = (2, 2) SG.
The construction we introduce, which is in essence based on general properties of Fierz identities, is in principle generalizable to higher dimensions and to higher extended supersymmetry. However, the specific topological background systems to which one has to couple the topological matter depend on the dimension and on the particular matter system one considers. For example, we found previously in [3] that the supersymmetric backgrounds of three-dimensional N = 2 supergravity were described by pure topological gravity. In the present paper we find instead that the topological description of localizations of twodimensional N = (2, 2) supergravity requires, beyond topological gravity, also a topological background abelian multiplet. At the moment, we do not have yet an a priori way to identify the correct topological gravity backgrounds which describe localizations of a given matter supersymmetric system: this remains an interesting open problem. We should also add that in our approach we are restricted to the case with at least two supercharges, which corresponds to backgrounds that satisfy a reality condition. This case is the one for which the complex conjugate of the (generalized) covariantly constant spinor is also covariantly constant. This is sometimes referred to as the real case in the literature.
The paper is organized as follows: In Section 2, we look for a topological counterpart of N = (2, 2) supersymmetric gauge theory which can be coupled to two-dimensional TG. To this end, we revisit the topological formulation of two-dimensional Yang-Mills (YM 2 ) theory [8] 3 , which forms the vector multiplet part of the matter SQFTs 4 . We end up with a topological version of two-dimensional standard YM theory coupled to a topological U (1) field strength background, which can be alternatively thought of as a twisted version of two-dimensional N = (2, 2) vector multiplet.
In Section 3, we find the consistent coupling of this matter topological YM theory to background TG. The resulting theory depends now on two topological backgrounds: the TG background and the topological U (1) field strength background. We also identify the associated BRST transformations for both matter fields and backgrounds which close offshell.
In Section 4, we classify the topological BRST invariant backgrounds. As it is familiar from SG, the BRST invariant topological backgrounds are specified by the BRST transformations rules for the backgrounds only: they are independent of the specific matter TQFT which couples to them. In the TG approach the equations which specify the invariant backgrounds are obtained by setting to zero the BRST variations of the two fermionic fields, i.e. the topological gravitino ψ µν and gaugino ψ (1) . The BRST variation of the topological gravitino of TG provides an equation for the metric and the bosonic ghost-for-ghost γ µ of the TG multiplet Simply put, these equations state that the ghost-for-ghost background is a Killing vector of the metric. In two dimensions, non-trivial solutions of (1.1) exist only if the euclidean spacetime manifold is either a 2-sphere S 2 or a 2-torus T 2 , equipped with a metric possessing at least one isometry V µ . Different topologies of the spacetime manifold only support the trivial solution γ µ = 0 which corresponds to the Witten topological twist [9]. The equation (1.1) is universal, in the sense that holds for any topological gravity system, in any dimension.
We mentioned above that in two dimensions we must consider a topological gravity system which includes also a topological U (1) multiplet background. Therefore, we obtain one more equation from the BRST variation of the topological U (1) background gaugino ψ (1) : where γ (0) is the bosonic superghost of the U (1) gauge multiplet background and f (2) is the U (1) field strength.
Eq. (1.2) is the simplest and most extensively studied example of equivariant cohomology: it states that the U (1) topological backgrounds (γ (0) , f (2) ) are equivariant classes of the S 1equivariant cohomology on the S 2 or T 2 euclidean spacetime. The interesting case is the one of the 2-sphere, S 2 . It is well-known that the S 1 -equivariant cohomology of the sphere is the polynomial ring generated by two classes x and y of ghost number 2, subject to the hypersurface relation We describe these classes in detail in Section 4. They parametrize the moduli space of inequivalent SG backgrounds that lead to supersymmetric localization.
In Section 5, we explain the map between BRST invariant backgrounds and localizing backgrounds of N = (2, 2) SG. This SG multiplet contains two graviphotons. The 2-form f (2) is identified with the field strength of one of them. The superghost fields -both the vector γ µ of TG and the scalar γ (0) of the topological U (1) gauge multiplet -which solve (1.1) and (1.2) coincide with the independent bilinears of the covariantly constant spinors of SG. In two dimensions, there is another scalar spinorial bilinear, c 0 , which is determined by the independent bilinears by means of a quadratic relation. This scalar bilinear turns out to be related, via an equation which is identical in form to (1.2), to the field strength G (2) of the second graviphoton: this second graviphoton of SG is therefore a "composite" field in terms of the topological variables. We will provide the explicit expression for the second graviphoton field strength in terms of the topological fields. Finally, we will also write down the field strength of the U (1) R -the R-symmetry of the supersymmetric matter theory -in terms of the topological backgrounds. In this way, all the bosonic fields of the SG multiplet which support generalized covariantly constant spinors are reconstructed in terms of the topological backgrounds solving (1.1) and (1.2).
In Section 6, we analyze in detail the case of the two-sphere S 25 . We recover all the known localizing solutions which have been described in the literature. We also uncover an infinite number of new solutions. The structure of the space of supersymmetric backgrounds is qualitatively different for vanishing and non-vanishing superghost background γ µ (x). When γ µ (x) = 0, our equations imply that the two graviphoton field strengths f and G are equal, f = G. We will see that this, in turn, forces the U (1) R field strength F R to coincide with half of the two-dimensional spacetime curvature R. These supersymmetric backgrounds correspond therefore to the old A-twisted topological matter models introduced by Witten long ago [9]. These backgrounds exists for any topology of the two-dimensional spacetime.
When γ µ (x) = Ω V µ (x) = 0, where V µ (x) the isometry of the sphere and Ω is the degree-two generator of the ring of S 1 -equivariant cohomology, the space of localizing backgrounds acquires new branches. In Figure 1 the supersymmetric solutions are labelled by the quantized fluxes (n, m) of the two graviphotons field stregths (f, G). The solutions with f = G and thus with F R = ± 1 2 R have now necessarily zero fluxes n = m = 0. These solu-tions, corresponding to the green dot of Figure 1, are the Ω-deformed sphere backgrounds of [6] and [7].
A non-vanishing superghost γ µ (x) also allows for solutions with f = G. If |n| = |m| the U (1) R flux is still ±1, but the spin connection cannot be identified with (twice) the U (1) R gauge field. These solutions, depicted in Figure 1 with red and blue dots, depend on a continuous parameter A -the zero-mode of the gauge scalar superghost γ (0)6 .
There is a second class of solutions with |n| = |m|, for which the zero-mode of γ (0) is discrete since it is identified with (half of) the flux m of the "composite" graviphoton. For these solutions m takes integer values in the set {−n, −n + 1, . . . , n}. These "discrete" solutions have U (1) R flux equal to zero. They are the black dots of Figure 1. The solution with n = −2 and m = 0 is the solution studied in [4] and [5].
We emphasize that the deformation parameter Ω is non-vanishing for all the solutions corresponding to the black, red and blu dots: in this sense we can say that these solutions all have non-trivial Omega-background since, in the topological gravity formulation, the natural definition of Omega-background is the vector superghost γ µ background. This definition includes the standard Omega-deformed S 2 as a particular case (the green dot) when the graviphoton field strengths are equal to each other. But it is more general and it applies to any spacetime dimensions since the form of the gravitino BRST variation of TG (1.1) is universal. For example, its relevance in three dimensions was discussed in [3]. In four dimensions, Nekrasov's Omega-deformation of twisted N = 2 super Yang Mills theory [10] is also captured by the superghost of the corresponding topological gravity. One should keep in mind that, because of ghost-number conservation, a non-trivial dependence of the partition function on the Omega background comes about only if one considers insertions of suitable operators carrying non-trivial ghost number. This poses an interesting and nontrivial lesson of our construction, applicable to any dimensions: in topological models, it is natural -and necessary to describe the full set of localizable SQFTs -to switch on topological backgrounds with non-vanishing and even ghost number.
In section 7, we describe the action of the non-compact SO(1, 1) duality group of SG on the localizing backgrounds. This non-compact duality group acts on the central charges of the supersymmetry algebra and it is an automorphisms of the generalized covariantly constant spinor equations [6]. In the topological framework, the duality group is the group of linear automorphism of the ring relation (1.3) which characterizes the BRST invariant backgrounds. The duality group is non-linearly realized on the topological backgrounds but it acts linearly on the cohomology classes x and y. It is in general broken by a given localizing background; however, discrete subsets of duality transformations map localizing SG backgrounds to different ones. We describe explicitly these discrete subsets for the various kind of localizing SG backgrounds in Section 7. In section 8, we summarize our main results and discuss issues which may be worth of future investigations.

A Topological Formulation of d = Yang-Mills Theory
The bosonic sector of two-dimensional N = (2, 2) supersymmetric gauge theory contains the YM 2 theory.
In this section, we develop a topological formulation of YM 2 theory, viewed as a deformation of topological YM 2 theory. We consider both theories defined on a smooth manifold Σ equipped with a metric g µν . The relation between standard YM 2 theory and topological YM 2 theory was investigated long ago in [8]. Witten's reformulation of YM 2 theory, although closely related to the topological theory, is not invariant under reparametrizations: it explicitly depends on a twodimensional metric g µν . Here, we revise Witten's formulation and obtain a matter TQFT which can be consistently coupled to TG.
Let us first review Witten's formulation of YM 2 theory, whose bosonic field content is identical to that of the topological counterpart: it consists of the gauge connection one-form field A = A a T a and a scalar field φ = φ a T a , both transforming in the adjoint representation of the gauge group G. T a , with a = 1, . . . dim G, are generators of the Lie algebra associated to the gauge group G. The theory's partition function is Here, I YM is the action functional where F is the field strength two-form Note that the -independent part of the action (2.4) coincides with the bosonic part of the action of the topological YM 2 theory. The partition function defines an effective action of the two-dimensional metric g µν and the deformation parameter .
The action (2.4) is invariant under the BRST gauge transformations s: The action I YM is quadratic in the scalar field φ which can therefore be integrated out, yielding the physical Yang-Mills theory action: Recalling that was initially introduced as a parameter that deforms away from the topological gauge theory, we see that it is identifiable with the coupling constant of the physical gauge theory. Conversely, the classical limit of the physical gauge theory is the topological gauge theory.
The theory (2.4) is neither invariant under diffeomorphisms nor under conformal transformations of the two-dimensional spacetime Σ(g). It is however invariant under area-preserving diffeomorphisms, w(∞), which span an infinite-dimensional symmetry transformations. This huge global symmetry is the basis for anticipating exact solvability of the theory [11], [12].
To further study how the infinite-dimensional global symmetry constrains the theory, we promote it to a local symmetry by coupling the theory to suitable background fields. Accordingly, we replace the volume-form √ g d 2 x with a topological background given by a two-form field f (2) . This changes the action (2.4) to This action does not have the same physical content as the original action. By Hodge decomposition, the two-form field f (2) takes the form where Ω (1) is a one-form and For I[f (2) ] to be equivalent to I YM [g, ], one must remove the degrees of freedom associated with Ω (1) . We can achieve this by letting the background f (2) transform under the BRST operator as follows where ψ (1) is a fermionic background of ghost number +1. However, the BRST transformation (2.9) is degenerate: we need therefore to further introduce a ghost-for-ghost background Since now the background field is not inert under s, the action (2.6) is no longer BRST invariant: To restore the BRST invariance, one must modify the BRST transformation law for the connection one-form A as We see that the BRST variation of the first term in I cancels the BRST variation of the second term: The problem with the modified transformation (2.12) is that it is no longer nilpotent: To fix this, it is necessary to modify also the BRST transformation rule for the ghost field c One finds that Moreover, an extra term in s 2 A cancels the term proportional to d γ (0) : Although this is still nonzero, the lack of nilpotency is now reduced to a term proportional to the equations of motion of A: We conclude that, on-shell, the BRST transformation for A is nilpotent: There is a systematic method to extend the on-shell BRST invariance to off-shell [3]. One starts by introducing a one-form field valued in adjoint representation of the gauge group G A ≡Ã a µ T a dx µ , carrying ghost number -1. One also modifies the BRST transformation rule for A by adding to it a term depending on the newly introduced one-form field A: This modification makes the BRST operator s nilpotent off-shell on all fields assuming that A transforms according to The term proportional to γ (0) in (2.13) spoils the BRST invariance of the action One needs therefore to further modify the action by adding to it a term quadratic in A, 14) The final action I, which is still topological, is manifestly invariant under BRST transformations acting on both the dynamical fields and the backgrounds Roughly speaking, we are introducing a set of spurion fields whose classical expectation values correspond to the backgrounds.
To construct a theory invariant under global topological supersymmetry, we consider the backgrounds which are fixed points of the BRST transformations (2.15): Given the Z 2 grading structure of the ghost number, one can choose the fixed point backgrounds to be purely bosonic: In these backgrounds, the BRST transformations act nontrivially only on the dynamical One can freely rescale the fields by the backgrounds to carrying ghost number 1 and 2, respectively. It is immediate to verify that the resulting theory is the quasi-topological Yang-Mills theory of [8].
At this point, it would be helpful to recapitulate the strategy we have paved so far.
Our starting point is YM 2 theory, which has the area-preserving diffeomorphisms as an infinite-dimensional global symmetry. To implement this global symmetry systematically, we first replaced the two-dimensional volume form by a two-form spurion field f (2) . The global symmetry of the original model is reflected by the fact that the action containing the spurion fields depends only on the cohomology class of f (2) . We showed that, as the background is promoted to a spurion field, this procedure entails both extending the BRST transformations to the spurion fields and accordingly deforming the BRST transformations of the gauge multiplet. This procedure amounts to promote the global symmetry to a local gauge symmetry. To ensure off-shell BRST invariance it was necessary to introduce an anticommuting one-form field, A, as a compensator. This field turned out to be proportional to the gaugino of topological YM 2 . We managed to obtain in this way a BRST invariant formulation of YM 2 theory coupled to topological spurion fields, viz. (f (2) , ψ (1) , γ (0) ).
A comment about the spurion topological multiplet (f (2) , ψ (1) , γ (0) ) is in order. The role of f (2) was to replace the metric volume form √ g d 2 x of the Witten formulation, as indicated in Eqs. (2.8) and (2.9). As such the topological spurion multiplet is not necessarily to be identified with the field strength multiplet of a U (1) topological connection. However we will see that, in the correspondence that we will establish between topological backgrounds and localizing SG backgrounds, f (2) will be identified with the field strength of one of the two SG graviphotons. Therefore it is natural to require that where a (1) is an abelian connection on Σ, which transforms under the BRST operator as follows: Here, ξ (0) is the ghost of the U (1) gauge symmetry.
The partition function which encodes the effective action of the spurion fields and hence the gauged global symmetry, satisfies the Ward identity This identity expresses the fact that the partition function depends only on the cohomology class of f (2) . In the BRST formulation, this is the statement that YM 2 theory is invariant under the area-preserving diffeomorphisms, viz. the w(∞) algebra.
Theories invariant under the 'rigid' topological supersymmetry are now obtained by restricting the spurion fields to the backgrounds which are bosonic fixed points of the deformed BRST operator, viz. γ (0) = constant and ψ (1) = 0, as explained in (2.16). Hence, there is a one-parameter family of theories, labelled by the BRST invariant constant background γ (0) .
Depending on the background value, the topological supersymmetry is realized differently.
For non-degenerate backgrounds, γ (0) = 0, one recovers the topological YM 2 theory and also identifies the topological gaugino ψ, which remained mysterious in Witten's formulation [8], with the "composite" spurion γ (0)Ã . As the background is non-degenerate, the standard YM 2 theory has the topological supersymmetry as a manifest symmetry. For degenerate background, γ (0) = 0, one recovers the original YM 2 theory (2.4). The topological supersymmetry collapses and the BRST symmetry reduces to the pure gauge one, (2.5). Thus, when γ (0) = 0, the topological supersymmetry can be thought of as a hidden symmetry of the standard Yang-Mills theory.

Coupling to d = 2 Background Topological Gravity
We next couple the TQFT constructed in Section 2 to two-dimensional TG. To this end, it is useful to formulate the theory in terms of superfields (or polyforms).
We introduce the dynamical superfields, both valued in the adjoint representation of the Lie algebra of the gauge group G: where φ is a two-form of ghost number −1 and c is a two-form of ghost number −2. The total fermion number is defined to be the sum of the form degree and the ghost number. So, A carries fermion number +1, while Φ carries fermion number 0. We also introduce the spurion superfield (whose expectation value yields the super-background) carrying total fermion number +2. One can show straightforwardly that the superfield where δ 0 stands for the derivation are equivalent to the BRST transformations (2.15) and also define the BRST transformations for φ and c: The BRST invariant action corresponds to the action (2.14). To see this, we solve for φ and c by putting into the action (3.22) and obtain the action (2.14).
We are ultimately interested in putting the theory on curved spacetime and in a background with nontrivial gauge fields. Therefore, we shall couple our topological formulation of YM 2 theory to two-dimensional TG. The field content of TG includes the metric g µν , the gravitino ψ µν , the diffeomorphism ghost ξ µ , and the ghost-for-ghost γ µ needed for the nilpotency of the BRST charge. They carry ghost numbers 0, 1, 1, 2, respectively. The BRST transformations of these fields [13] are where L ξ is the Lie derivative associated with the vector field ξ.
It is useful to introduce the operator S S ≡ s + L ξ which satisfies the relation on all the fields except the vector field ξ µ . Finding a nilpotent BRST operator s for the matter TQFT coupled to TG is equivalent to finding an operator S that satisfies the relation (3.24) on the matter sector. The solution to this problem [14] is obtained by replacing the coboundary operator δ 0 with a new nilpotent operator δ: in the transformations rules (3.21): The equations above describe the BRST transformation rules for topological YM 2 theory coupled to TG. In components, these transformations become Most importantly, the action (3.22) remains BRST invariant even when the spacetime manifold Σ is curved. In general, we can add to the action terms of the form I n = a n n Σ f Tr Φ n , (n = 2, · · · ) . (3.28) In particular, in case the gauge group G contains U (1) factors, we can add a topological counterpart of the Fayet-Iliopoulos term which, after eliminating φ and c, becomes For n = 2, we regain the BRST invariant action (3.22).

BRST invariant Topological Backgrounds
Having coupled the matter TQFT to TG, we now look for the background configurations that are BRST invariant. The BRST invariance conditions for the fermionic fields of both TG and topological U (1) multiplet read S ψ µν = 0 and S ψ (1) = 0.
They lead to the equations characterizing the backgrounds in correspondence of which the matter QFT acquires global topological supersymmetry. Our aim is to solve these equations and classify the solutions modulo BRST trivial ones.
The action depends on the topological backgrounds only through the BRST operator S. The BRST operator, in turn, depends on the ghost-for-ghost γ µ of TG and on the U (1) fields γ (0) and f (2) only. Therefore, when the equations (4.30) are satisfied, the matter QFT is automatically independent of any variation of the metric that preserve γ µ , as well as of any topological variation of the U (1) fields that preserve the class of f (2) .
The first equation in (4.30) asserts that the ghost-for-ghost γ µ has to be a Killing vector of the two-dimensional metric g µν . This equation takes the same form in any spacetime dimensions, but the moduli space of solutions differs. In the context of three-dimensional supersymmetric gauge theories, its moduli space was discussed in [3]. In two dimensions, it is well-known that there are Killing vectors on the sphere S 2 and on the torus T 2 , but not on higher-genus Riemann surfaces. Given the Killing vector γ µ , we conclude that the matter QFT is independent of any γ-invariant deformations of the metric. Generically, these metrics have only a U (1) isometry. This is the case for example for the squashed two-sphere S 2 q studied in [15] and [6]. Given the Killing vector γ µ , we now turn to study the equations for the U (1) gauge field background. The consistency of (4.30) requires This means that all the backgrounds g µν , f (2) and γ (0) must be L γ -invariant. Trivial solutions are of the form where θ (1) is a globally defined L γ -invariant 1-form: provided we make the identifications where V is the Killing vector associated with the S 1 -equivariant action and Ω is the degreetwo generator of the ring of the S 1 -equivariant cohomology. The f (2) + Ω f (0) , which appears in (4.32), is the equivariantly closed extension of the ordinary differential form f (2) and d − Ω i V is the Cartan differential.
For Σ = S 2 , it is well-known that there are two linearly independent equivariant classes x and y of degree-two 7 . The first class is the ring variable itself: x = Ω . 7 We present an elementary proof of this assertion in the Appendix B.1.

The second class is
Here, f (0) is solved only up to an additive constant: given a choice of this constant, a shift to another value induces the change y → y + c x .
We choose the normalization of the variable y such that where N is one of the fixed points of the vector field V . If S is the other fixed point of V , we can choose The localizing SG background found in [4] corresponds to an equivariant class of the form a y + b x with a = 0, whereas the background identified in [7] corresponds to a class with a = 0. The square of y is an equivariantly closed class of degree-four: Hence, we have from which we derive the cohomological equation Here, α and β are determined by With the normalizations (4.33) and (4.34), we have We thus obtain the cohomological relation which tells us that the S 1 -equivariant cohomology at any degree is the polynomial ring generated by x and y modulo the relation (4.35).
Throughout the above analysis, we were taking both the TG backgrounds and the U (1) field strength f (2) background to be real-valued. This implies that, for Σ a compact surface, the flux of f (2) must be quantized. Hence, on the two-sphere, the relevant cohomology is the integer valued S 1 -equivariant cohomology. In Section 6.1, we will discuss the impact of this quantization condition on the topological moduli space.
For Σ = T 2 , the S 1 -action is free. So, the equivariant cohomology is the same as the standard cohomology of the quotient T 2 /S 1 S 1 8 . As such, there is just one parameter for the inequivalent BRST invariant topological backgrounds.

Relation to Supergravity Backgrounds
Given the classification of the topological backgrounds just discussed, our next goal is to establish a map between the topological BRST invariant backgrounds and the supersymmetric backgrounds of two-dimensional N = (2, 2) SG. We will show that the equations determining the BRST invariant topological backgrounds which we derived in the previous Section are equivalent to the equations for the generalized covariantly constant spinors of N = (2, 2) SG in two dimensions. It will be clear from our discussion that the method we will explain is very general, and it can be applied to other dimensions or to higher supersymmetry contents. We expect that the topological system which describe localizing backgrounds of SG with higher supersymmetry and/or in higher dimensions will include more topological gauge multiplets beyond the single abelian one which we considered in this paper.
The localizing backgrounds of SG are determined by the generalized Killing spinor equation, which is obtained by requiring the vanishing of the supersymmetry variations of the gravitino [6]: Here, the covariant derivative D µ includes the spin connection associated with the frame rotation on the tangent space T Σ, the vector field A µ is the U (1) R gauge field minimally coupled to the R-symmetry current, and the scalar fields H and G are the Hodge duals of the two graviphoton field strengths. The cases with at least two supercharges of opposite R-charges are the ones discussed in the previous works since they lead to amenable computations. They correspond to backgrounds in (5.36) which satisfy the following reality For these backgrounds, the conjugate of (5.36) reads

Graviphoton Backgrounds
The map between the TG backgrounds and the SG backgrounds is obtained by considering the decomposition of the bi-spinor in two dimensions:

The Fierz identities in two dimensions lead to the relation
where we raised the indices of c µ using the background metric g µν . The equations (5.36) and (5.38) for the spinors ζ and ζ † imply the following equations for the bilinears c 0 , c µ , c 0 where we used the relation The SG variables H, c µ , and c 0 have to be identified with the topological background fields according to the following map: Therefore, in correspondence to a solution of the topological equations we can construct a solution of the equations (5.40), which is defined by together with Eqs. (5.41).
As explained in the previous Section, solutions of the topological equations (5.42) that are related by the transformations varies by where Moreover, Hence we conclude that, under the gauge transformations (5.44), the "composite" fields G (2) and c 0 transform in the same way as the topological fields f (2) and γ (0) : In particular, is invariant under the BRST transformations, provided that the backgrounds satisfy the BRST invariance equations (5.42).

U (1) R Field Strength Background
We have seen how the topological backgrounds specify the spinorial bilinears and thus the backgrounds H and G. Below, we show how the U (1) R field strength is also obtained from the same topological backgrounds.
From the equation for the generalized covariantly constant spinors: Antisymmetrizing with respect to µ, ν yields Hence, we arrive at the equation Nontrivial solutions of this equations exist whenever For generic f and G, (5.49) would require that F R be complex-valued. However, since the fluxes are annihilated by the Lie derivative along γ: and thus the square of the field strength, F 2 R , is real-valued: As a matter of facts, not only the square but also F R itself is real. This can be understood as follows. We first rewrite the integrability condition (5.48) in a different form. From (5.47), we have Since f and G are L γ invariant, the imaginary terms in the equations above drop out: This can be proven as follows. γ µ D µ f = 0 implies . The same holds for G. It then follows immediately that √ g µν D µ G D ν f = 0.
Combining the two equations, we obtain a manifestly real-valued expression of the U (1) R field strength The flux of F R does not necessarily vanish since the vector field becomes singular at the zeros of the vector field γ µ . If we perform the transformation (5.44) on f and γ (0) , the field strength F R changes by a globally defined total derivative: which implies that the flux of F R is invariant under topological transformations.
From (5.51), we can also express the scalar spinorial bilinears in terms of the SG backgrounds: We note that the field strength background (5.50) encompasses all known backgrounds discussed in [6] as special cases. When (5.50) is satisfied, the matrix in (5.47) is generically of rank-one. In this case, the system has only two global supercharges. The system has four global supercharges when the matrix has rank-zero, that is when the U (1) R field strength vanishes, which agrees with the results of [6].
Let us also observe that Eq. (5.50) implies that whenever We might take this as the definition of the A-model, whose twisting was indeed originally characterized by identifying the spin-connection with twice the U (1) R gauge field.
From Eq. (5.43) we see that γ µ = 0 automatically implies the A-model condition (5.53): the corresponding backgrounds -i.e. γ µ = 0, f = G and F R = ± 1 2 R -identify the old A-model introduced by Witten in [9]. When instead the A-model condition (5.53) is satisfied by γ µ = 0 one obtains the so-called [6] Ω-deformed A-model on the sphere. We will verify this in detail in subsection 6.2.

Classification of Supergravity Backgrounds
Our considerations in earlier sections apply to any two-dimensional spacetime Σ equipped with a metric which has an isometry. In this Section we shall focus separately on Σ = S 2 and T 2 . While non-compact Σ = H 2 is an equally interesting case, due to new features, we shall relegate its study to a separate work. As we explained in the previous sections, there is no loss of generality in taking the metrics on S 2 and T 2 be maximally symmetric.

All Supersymmetric Localizing Backgrounds on S 2
Consider the round two-sphere S 2 with coordinates ds 2 = dθ 2 + sin 2 θ dφ 2 . (6.55) We take γ µ to be proportional to one of the three Killing vector fields, Up to topological equivalences, we know that the general solution of (5.42) is given by where A is a constant and n ∈ Z labels the first Chern class of the topological connection The modulus A for a generic solution which is topologically equivalent to (6.57) can be expressed as This expression is topologically invariant since the Killing vector γ µ vanishes at the poles of For the graviphoton background G, we obtain , (6.60) whose flux takes the value Therefore, by requiring the quantization of this flux, we see that, when |A| ≥ |n| 2 , A is a continuous moduli parameter of this family of solutions. On the other hand, when |A| < |n| 2 , the quantization of the flux for G imposes that A be a discrete parameter, taking the 2 n − 1 values The U (1) R field strengths corresponding to the topological backgrounds (6.57) are The flux of U (1) R gauge field is then given by

Ω-Deformed S 2
In this Section we will focus on the solution with n = m = 0 (the green dot of Figure 1): F R is given by Eq. (5.50) and its flux is +1 (−1) if A > 0 (A < 0) 11 . In this subsection we show that this background is topologically equivalent, in the sense of Eq. (5.44), to the so-called Ω-deformed S 2 . The Ω-deformed A-model was defined in [6] and [7] by the equation We have already remarked that this equation implies the identification of the F R with half of the world-sheet curvature. By substituting Eq. (6.69) into (5.43), one obtains the equation Taking account of (5.42) and (6.55), this gives which can be easily solved to yield one verifies that the Ω-deformed background (6.72) is indeed topologically gauge equivalent to i.e. to the background (6.57) with n = 0 and A = − 1 2 B . In our considerations so far, both G and f are taken real-valued. There actually exists another class of consistent SG backgrounds for which both G and f are purely imaginaryvalued. Formally, these backgrounds can be obtained from our backgrounds by analytically continuing our formulas to pure imaginary values of A. The background with A = i, for example, is the situation discussed in [5]. For this "Wick-rotated" backgrounds, the twodimensional flux configurations of the backgrounds correspond to exchanging n and m in

All Localizing Backgrounds on T 2
For Σ = T 2 , let us adopt the coordinates ds 2 = dθ 2 1 + dθ 2 2 . (6.74) We choose the vector field γ to be one of the two Killing vectors: Up to topological equivalences, the general solution of (5.42) is given by We see that the allowed values for the background fields are considerably reduced compared to those for S 2 . This is because the first Chern class of the topological U (1) gauge field must vanish.

O(1, 1) Duality Symmetry
In this section we will show that some of the duality automorphisms of the supersymmetry algebra act as solutions generating symmetries. To see this, let us return to the Killing spinor equation where On a compact surface Σ, the fluxes of f and G must be quantized. In general, given a background configuration of (7.77) with quantized fluxes, the configuration obtained after the duality transformations (7.78) may not have quantized fluxes. When this happens, the transformed background is not physically acceptable. This implies that, for compact manifolds, the continuous duality symmetry O(1, 1; R) is generically broken.
Still Take first the solutions with |A| > |n| 2 > 0 which have f and G fluxes equal to (n, m) = (n, ±n). We will focus on the n > 0 and m = n class of background configurations, as the foregoing analysis would similarly hold for other classes. From (7.82), we see that the duality transformations which act on such backgrounds form a subgroup isomorphic to Z, whose elements are the matrices for which e α k = k, equivalently, α k = log k + 2πiZ (7.83) for some k positive integer such that Under such discrete duality transformation, the moduli A and n of the backgrounds are transformed to We see that, starting from the solutions with n = 1 and all A > 1/2, one can generate all other solutions with n > 0 and A > n/2 by O(1, 1; R) duality transformations.
On the other hand, generic discrete solutions for A = m 2 and fluxes (n, m) with |m| < |n| and n = 0 breaks completely the O(1, 1; R) duality symmetry group (7.78). This is the case, for example, of the solution (n, m) = (−2, 0) of [4], since the only solution of the Ω-deformed S 2 By a general O(1, 1; R) rotation, one obtains (γ (0) ) Ω = sinh α sin 2 θ + A 2 + cosh α A (7.86) and hence that We see therefore that, starting from the n = 0 A = 1 model, one obtains all values A > 0 by acting with the duality symmetry transformation. Summarizing, the O(1, 1, R) duality transformations generate, starting from the solutions with n = ±1 and n = 0 in the continuous branch, all other solutions with generic n and A continuous. On the other hand, the solutions in the discrete branch, with A = m 2 and |m| < |n| are, generically, not connected by the duality transformations. The action of the duality transformations on the localizing SG backgrounds is depicted in Figure 2.  Figure 2: The action of the discrete non-compact duality symmetry on fluxes:

Conclusions
In this work, we have obtained a complete classification of supersymmetric localizing backgrounds (metric and gauge field) that can be constructed in two-dimensional N = (2, 2) SG.
The key idea has been to couple two-dimensional matter TQFT to topological gravity and to relate BRST invariant topological backgrounds to supersymmetry preserving SG backgrounds. This approach was already introduced in three dimensions in [3]. The present work discusses its universality and generality and also explicitly works out the dictionary between the TG and SG approaches in two dimensions.
Unlike the SG approach widely discussed in the literature, our analysis uses TG to analyze and classify the manifolds admitting generalized covariantly constant spinors. In this paper, we showed that all the two-dimensional backgrounds which admit generalized covariantly constant spinors can be obtained via TG. More precisely, we demonstrated that there is a precise map which allows to reconstruct, given a BRST invariant topological background, a solution of the equations for generalized covariantly constant spinors in N = (2, 2) SG. From a more technical point, we have learned that the two-dimensional case presents a new feature when compared to the three-dimensional one analyzed in [3]: one needs to introduce also a background U (1) topological gauge field, equivariantly coupled to TG. In Section 2 we have shown that the abelian gauge multiplet is necessary to consistently couple the YM 2 theory to TG. In other words, the rigid matter theory explicitly tells us what are the backgrounds which need to be introduced.
In fact, the topological approach also provides a natural and precise notion of equivalent backgrounds, i.e. backgrounds that can be made equal through topological gauge transformations. In this way, it becomes much easier to obtain a complete classification of the localizing backgrounds. We believe this is a significant advantage over the more traditional SG approach, for which the analogous notion has not yet been worked out.
The natural implication of our map is the prediction that the topological partition func-  We found many more supersymmetric localizing solutions than those that have been explored so far: it would be interesting in particular to investigate the "discrete" solutions that generalize the one of [4] and [5]. In this regard, it would be also interesting to understand how the non-compact duality transformations act on the partition functions of different supersymmetric localizing backgrounds.
A direction for future investigation might be the uplift of the new supersymmetric localizing backgrounds we discovered to the superstring setup. The two-dimensional matter SQFTs with at least 2 supercharges contain vector, chiral and twisted chiral supermultiplets. Such systems arise as the low-energy limit of two-dimensional matter on intersecting D-branes. It could be interesting to study how the topological symmetry which we have uncovered is realized from the brane perspectives.
Another direction is to understand better the Ω-deformation. We related this background to turning on the background of vector superghost in TG. It would be interesting to extend this to the most general Ω-deformations and to utilize the two-dimensional analysis in this paper to the worldsheet formulation of the Ω-deformations.
As yet another direction, we note that the coupling of the matter TQFT to TG is also the starting point for constructing topological strings. It seems reasonable to ask if the backgrounds with non-vanishing ghost number which were at the core of our analysis are relevant in the topological string set up in which the topological backgrounds become dynamical. One might speculate that the Ω-deformation be relevant to the world-sheet understanding of the refined topological string, in particular, in the context of computation of elliptic genera of M-strings in six dimensions [16], [17], [18], and monopole strings in five dimensions [19], [20].
We hope we made clear that the methods introduced in this paper are quite general and they are not restricted either to two dimensions or to N = (2, 2) SG: we believe they might be a valuable tool to explore localizing backgrounds also in other dimensions and with different supersymmetry content. For example, it should be relatively simple to study localizing backgrounds which arise in two-dimensional N = (4, 4) SG 13 .

A Standard YM Theory from Topological YM Theory
We asserted that, in two-dimensional spacetime, standard YM theory is related to topological YM theory by a certain deformation. Here, we explain details of this relation. The starting point is the partition function of the standard YM theory, viewed as a deformation of the topological YM theory: where · · · top denotes the vacuum expectation value computed in the topological YM theory.
Since we are expanding in , Z pert ( ) is of course only the perturbative part of the full partition function Z( ) of the standard theory: Z pert ( ) does differ from Z( ) by exponentially small, nonperturbative terms of O e − 1 .
One also observes that the zero-form Using the same orthogonal decomposition as in (B.103) for θ (1) , ω (0) and h (1) , we now obtain L γ θ (1) = L γ θ and f (2) is reduced to However, there is no nontrivial U (1) bundle on T 2 invariant under γ. We must therefore set