Simplified pure spinor b ghost in a curved heterotic superstring background

Using the RNS-like fermionic vector variables introduced in arXiv:1305.0693, the pure spinor b ghost in a curved heterotic superstring background is easily constructed. This construction simplifies and completes the b ghost construction in a curved background of arXiv:1311.7012.


Introduction
Although the pure spinor formalism for the superstring [1] has several nice features such as manifest spacetime supersymmetry and a simple BRST operator, a complicated feature of the formalism which needs to be better understood is the pure spinor b ghost. Unlike in the bosonic string or Ramond-Neveu-Schwarz (RNS) string where the b ghost is a fundamental worldsheet variable, the b ghost in the pure spinor formalism is a composite operator constructed from the other worldsheet variables.
The BRST operator Q in the pure spinor formalism is independent of the target-space background and takes the simple form Q = dz (λ α d α + ω α r α ) (1.1) where (λ α , d α , ω α , r α ) are fundamental worldsheet variables. To satisfy the relation {Q, b} = T where T is the conformal stress tensor, b was constructed in a flat background in [2] as a complicated function of the worldsheet fields. This construction of the pure spinor b ghost was simplified in [3] by introducing a fermionic vector field Γ a which was related to the usual RNS fermionic vector field ψ a by "dynamical twisting". An important question is how to generalize this construction of the pure spinor b ghost in a curved superstring background. In [4], the pure spinor b ghost was constructed in a super-Maxwell background of the open superstring, and in [5], the pure spinor b ghost was constructed in an N=1 supergravity background of the heterotic superstring. The construction in [5] for a curved heterotic superstring background was quite complicated and some of the coefficients of the composite operator for the pure spinor b ghost were not explicitly computed.

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In this paper, we will use the RNS-like fermionic vector field Γ a of [3] to simplify the construction of the pure spinor b ghost in a curved heterotic superstring background. When expressed in terms of Γ a , the composite operator for the pure spinor b ghost in a curved heterotic background is a simple covariantization of the composite operator in a flat background that was found in [3]. In addition to simplifying the construction in a curved heterotic background, it is hoped that this method involving Γ a will also be useful for constructing the pure spinor b ghost in an N=2 supergravity background of the Type II superstring.
In section 2, we review the pure spinor formalism of the heterotic superstring in a flat and curved target-superspace background. In section 3, we define the RNS-like variable Γ a in a curved background. And in section 4, we use Γ a to explicitly construct the pure spinor b ghost in a curved heterotic superstring background. The appendix computes the BRST transformations of Γ a and the b ghost in a flat background.

Review of the non-minimal pure spinor formalism
In this section we review the non-minimal pure spinor formalism of the heterotic superstring in flat space [2] and in a curved background [5].

Non-minimal pure spinor formalism in flat space
The non-minimal pure spinor formalism in the heterotic superstring is constructed using the ten-dimensional N = 1 superspace coordinates (X a , θ α ) for a = 0 to 9 and α = 1 to 16, the conjugate variable of θ α which is called p α , a set of pure spinor variables λ α , λ α , r α together with their conjugate variables (ω α , ω α , s α ), and the same 32 fermionic right-moving variables ξ R for R = 1 to 32 as in the RNS heterotic superstring formalism. The pure spinor variables are constrained to satisfy (λγ a λ) = λγ a λ = λγ a r = 0 , where (γ a ) αβ and (γ a ) αβ are the symmetric gamma matrices which satisfy the Dirac algebra Because of the pure spinor conditions (2.1), the conjugate pure spinor variables are defined up to the gauge invariances where Λ 1 , Λ 2 , Λ 3 are arbitrary gauge parameters. The action of the theory is quadratic in these variables and is given by is the minimal pure spinor action.

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The quantization of this system is performed by introducing a left-moving BRST charge given by This BRST charge is nilpotent because of the OPE The BRST transformations of the worldsheet fields of our system are Note that the non-minimal sector in our system does not change the cohomology of the minimal sector and the action (2.4) can be written as The non-minimal pure spinor formalism does not contain the (b, c) worldsheet reparameterization ghosts. However, one can construct an operator b satisfying the equation Qb = T where T is the world-sheet stress tensor of the action (2.4), and this operator is identified with the pure spinor b ghost [2]. It was shown in [3] that this b ghost is simplified by introducing the RNS-like fermionic vector where N ab = 1 2 (λγ ab ω) is the Lorentz current for the minimal pure spinors. In terms of (2.12), the pure spinor b ghost is To verify the relation Qb = T , we first compute the action of Q on Γ a to be 14) The proof of (2.14) and the verification of Qb = T in a flat background are in the appendix. The purpose of this paper is to find a Γ a in a curved heterotic superstring background that satisfies an equation analogous to (2.14) and to define the b ghost as the covariantization of (2.13). In order to do this, we will need the BRST transformations corresponding to (2.10) in a curved background. We now review the non-minimal pure spinor formalism in a curved heterotic superstring background.

Non-minimal pure spinor formalism in a curved background
The minimal sector of the heterotic string in a curved background was constructed in [6]. The action has the form the graded-antisymmetric two-form superfield, Φ is the dilaton superfield which couples to the two-dimensional worldsheet curvature r, where T RS I are the SO(32) adjoint matrices for I = 1 to 496 and A I M , W Iα , F Iab are the super-Yang-Mills gauge fields and field-strengths, and where the connection Ω Aβ α has the structure Here Ω Aab is the usual Lorentz connection and Ω A is a connection for scaling transformations introduced in [6], and one can verify their coupling preserves the pure spinor gauge invariance of (2.3). The presence of the scale connection Ω A in (2.15) implies that the action is invariant not only under the usual local Lorentz transformations, but also under the local fermionic scale transformations So variables and superfields with raised tangent-space spinor indices carry charge +1 with respect to the fermionic scale transformations and variables and superfields with lowered tangent-space spinor indices carry charge −1.
The minimal BRST charge is given by Q 0 = λ α d α and it was shown in [6] that nilpotency and holomorphicity of Q 0 forces the background to satisfy the equations of N = 1 ten-dimensional supergravity. Nilpotency implies that where T αβ A and R αβγ δ are torsion and curvature components. And as shown in [6], nilpotency and holomorphicity imply that the torsion components can be gauge-fixed to the form T αβ a = γ a αβ , T Aβ

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In addition, the absence of chiral [6] and conformal [7] anomalies of the worldsheet action implies that Ω α is related to the dilaton superfield Φ by The BRST transformations of the minimal fields in (2.15) were determined in [8] to be where the first term in these transformations is a Lorentz and scale transformation proportional to λ β Ω βγ α .
For the non-minimal sector, it was noted in [5] that there is an effect of the background geometry on the BRST transformations of the non-minimal pure spinor fields. Assuming that the minimal sector is unaffected by the non-minimal variables, a cohomological argument determined that λ, ω, r, s transform in a curved background as Note that the torsion T γab includes the Lorentz connection Ω γab , so the Lorentz part of the spin connection of (2.18) does not appear in these non-minimal BRST transformations.
To construct the non-minimal action in a curved background, the BRST-trivial term S non−min = Q d 2 z s∇ λ + 1 4 Π A T Aab sγ ab λ (2.25) will be added to the minimal action of (2.15) where ∇ λ α = ∂ λ α − λ β Π A Ω Aα β . This construction is analogous to the flat action of (2.11), and although the torsion term in (2.25) is not needed for covariance and was not included in [5], it will simplify the construction by decoupling the Lorentz connection Ω Aab from the non-minimal action. Using the BRST transformations of (2.24), one finds that where we have used the Bianchi identity in the second line of (2.26).
Using the Noether method, one can easily determine the BRST charge corresponding to the action of S = S 0 + S non−min to be Q = dz (λ α d α + ω α r α ) . (2.29) 3 Definition of Γ a in curved background

Simplified BRST transformations
The first step in defining the curved background generalization of Γ a of (2.12) is to define a new variable In terms of D α , the BRST transformation of ω α is given by where we have used that Q(λΩ) = 0 because Ω α is proportional to ∇ α Φ. To prove that the second line in (3.3) is zero, symmetrize in (βγ) and use the Bianchi identity R (αβγ) δ = 0 and λ β λ γ R βγ = 0 to show that the second line is equal to

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It will be useful to defineQ = Q − Q L+S where Q L+S is this Lorentz and scale transformation, and one finds that where we have used that

Construction of Γ a
In this subsection, it will be shown that satisfies the BRST transformatioñ whereQ is defined in (3.5). Comparing with the equations of (2.12) and (2.14), one sees that (3.7) is constructed in a curved background by replacing d α in the flat-space construction with D α of (3.1).

JHEP06(2014)001 4 Definition of b ghost in curved background
In this section, we will use the dynamical twisting method of [3] to simplify the construction of the b ghost in a curved heterotic background which was proposed in [5]. We will show that the b ghost in a curved background can be defined in terms of the dynamically twisted RNS-like variable (3.7) by simply covariantizing the flat-space expression of (2.13) as (4.1) As in the action of (2.25), the torsion term in (4.1) is not needed for covariance and was not included in [5], but simplifies the construction by removing the dependence of the b ghost on the Lorentz connection Ω Aab .
To prove that Qb = T where T is the stress-energy tensor of the heterotic string in a curved background, note that S = S 0 + S non−min of (2.15) and (2.25) implies that

(4.2)
So one needs to show that where we have used that Γ a of (3.7) transforms as δΓ a = −2ΛΓ a . Using the definition ofQ = Q − Q L+S in (3.5), (4.3) is therefore implied if (4.6) Because of the similarity of (3.5) with the flat space BRST transformations of (2.10) and the result that Q flat b flat = T flat , proving (4.6) only requires showing that the various factors of (λ α Ω α ) coming from (3.5) and (3.8) cancel out in (4.6). The first term in (4.4) contributes no factors of (λ α Ω α ) and the second term in (4.4) contributes −2(λΩ)Π a Γ a from theQ variation of Γ a . The third term in (4.4) contributes

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where the first term comes from the variation of (λ λ) −1 , the second term from the variation of λ α , and the third term from the variation of Γ a Γ b . Finally, the fourth term in (4.4) contributes − 1 2 λ λ 2 5(λΩ) λ λ ωγ a λ (λγ a Π) + 1 2 λ λ 3(λΩ) ωγ a λ (λγ a Π) (4.8) where the first term comes from the transformation of (λ λ) −1 , the second term comes from the transformation of ω α , the third term comes from the transformation of λ α , and the last term comes from the transformation of Π α . To show that (4.8) is zero, we have used that So we have proven that the (λΩ) factors cancel out in (4.6), and therefore Qb = T .

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which is the term linear in r in (2.14). To go from the first line to the second line of (A.2), we have used the identity together with the pure spinor constraints of (2.1). Finally, the terms quadratic in r in (A.1) are which is the term quadratic in r in (2.14). To go from the first line to the second line of (A.4), we have used the identity r α r β = 1 96 γ def αβ (rγ def r). To go from the second line to the third line, we have used that λγ b α N bc = 1 2 J(γ c λ) α where J = −λ α ω α and that all terms proportional to J vanish using the pure spinor constraints of (2.1). And to go from the third line to the fourth line, we have So we have proven that Γ a satisfies equation (2.14) in a flat background.
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