Supersymmetric geometries of IIA supergravity III

We find that (massive) IIA backgrounds that admit a G2⋉ℝ8\documentclass[12pt]{minimal} \usepackage{amsmath} \usepackage{wasysym} \usepackage{amsfonts} \usepackage{amssymb} \usepackage{amsbsy} \usepackage{mathrsfs} \usepackage{upgreek} \setlength{\oddsidemargin}{-69pt} \begin{document}$$ {G}_2\ltimes {\mathbb{R}}^8 $$\end{document} invariant Killing spinor must exhibit a null Killing vector field which leaves the Killing spinor invariant and that the rotation of the Killing vector field satisfies a certain g2 instanton condition. This result together with those in [4] and [5] complete the classification of geometries of all (massive) IIA backgrounds that preserve one supersymmetry. We also explore the geometry of a class of backgrounds which admit a G2⋉ℝ8\documentclass[12pt]{minimal} \usepackage{amsmath} \usepackage{wasysym} \usepackage{amsfonts} \usepackage{amssymb} \usepackage{amsbsy} \usepackage{mathrsfs} \usepackage{upgreek} \setlength{\oddsidemargin}{-69pt} \begin{document}$$ {G}_2\ltimes {\mathbb{R}}^8 $$\end{document} invariant Killing spinor and where in addition an appropriate 1-form bilinear vanishes. In all cases, we express the fluxes of the theory in terms of the geometry.


Introduction
It has been known for some time that the maximally supersymmetric backgrounds of standard IIA supergravity are locally isometric to Minkowski space, while massive IIA supergravity does not admit such solutions [1]. Furthermore, it has been shown in [2] that there are no IIA solutions that preserve strictly 31 supersymmetries following a similar proof for IIB in [3]. On the other end, there are locally four different types of IIA backgrounds preserving one supersymmetry distinguished by the isotropy group of their Killing spinor in the local gauge group Spin (9,1). The geometry of the backgrounds with isotropy groups Spin (7), Spin(7) ⋉ R 8 and SU (4) have been investigated in [4,5]. The purpose of this paper is to examine the geometry of the remaining backgrounds, which admit a Killing spinor with isotropy group G 2 ⋉ R 8 . The combined four cases give a complete description of the local geometry of all (massive) IIA backgrounds that preserve one supersymmetry. The methodology we use to solve the Killing spinor equations (KSEs) of IIA supergravity is that of spinorial geometry proposed in [6]. For this we choose a representative of the G 2 ⋉ R 8 -invariant Killing spinor as ǫ = f (1 + e 1234 ) + g(e 1 + e 234 ) , (1.1) where f and g depend on the spacetime coordinates, see appendix A for an explanation of our spinor notation. If either f or g vanishes, then the isotropy group of ǫ becomes Spin(7) ⋉ R 8 and such solutions have already been investigated in [4]. Because of this we take that neither f nor g vanishes on the patch where the KSEs are investigated. Then this spinor is substituted into the KSEs, which turn into a linear system for components of the fluxes and the spin connection, which encodes the geometry. The solution of the linear system expresses some of the fluxes in terms of the geometry and also gives the conditions on the geometry for a background to admit such a Killing spinor.
In particular, we find that all backgrounds for which (1.1) is a Killing spinor satisfy the following geometric conditions Therefore, such backgrounds admit a null 1-form spinor bilinear e − such that the associated vector field K is Killing and leaves invariant the Killing spinor ǫ; for more details on the definition of e − see appendix A. These two conditions have been expected as they follow

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from the properties of the symmetry superalgebra for supersymmetric backgrounds, 1 see e.g. [7]. In addition, the rotation de − of K is restricted to be a section of a bundle Λ ′ 7 ⊕ I ⊕ Λ 14 which will be defined in section 2.3, and which can be interpreted as a g 2 instanton condition with an additional null component. Furthermore, the geometry of spacetime satisfies two more mild geometric conditions given by (2.19) and (2.20). The latter can also be interpreted as expressing the dilaton Φ in terms of the geometry.
There is a special subclass of G 2 ⋉ R 8 backgrounds which is characterized by the additional condition that a certain 1-form bilinear vanishes. It turns out that the IIA backgrounds admit two 1-form bilinears κ(ǫ, ǫ) and κ(ǫ, Γ 11 ǫ), and that where h is a spacetime function and κ(ǫ, ǫ) is the bilinear associated with the Killing vector field K. The requirement that κ(ǫ, Γ 11 ǫ) vanishes leads to the condition that h = 0 which in the gauge (1.1) implies that f 2 = g 2 . In this special case, the conditions on the geometry are as in (1.2) and (⋆ϕ, dϕ) = 0 , where ϕ is the fundamental G 2 3-form and ⋆ϕ is its dual as defined in appendix B. This vanishing condition is well-known as it implies that one of the classes in a Gray-Hervella type of classification of manifolds with G 2 structure vanishes [8,9]. There is an additional geometric condition given in (3.4), which is the analogue of (2.20) for the special case. Again this can also be interpreted as a condition on the dilaton. Furthermore, the expression of the fluxes in terms of the geometry dramatically simplifies. The description of the geometry we have given is local, i.e. it assumes that the Killing spinor can always be brought into the form (1.1) up to a local Lorentz transformation. Generically, solutions of the KSEs are not required to preserve the isotropy group of the Killing spinors in Spin(9, 1) everywhere on the spacetime. As a result there may be backgrounds which (globally) admit Killing spinors whose isotropy groups differ between different patches. Furthermore, as the rank of the IIA spin bundle is 32, and thus much larger than the dimension of the spacetime, the mere existence of a non-vanishing spinor does not reduce the structure group of the spacetime. 2 Of course if one asserts that the isotropy group of the Killing spinor is the same everywhere on the spacetime, then the structure group reduces to a subgroup of the isotropy group. However, this is an additional assumption.
This paper has been organized as follows. In section 2, we summarize the KSEs of (massive) IIA supergravity and describe the solution of the linear system, for all backgrounds admitting a G 2 ⋉ R 8 -invariant Killing spinor, for both the fluxes and geometry. In section 3, we investigate the geometry of the special class of backgrounds for which the aforementioned 1-form bilinear vanishes. In section 4, we give our conclusions. In JHEP06(2016)045 appendices A and B, we explain our spinor notation, describe various formulae which are useful for the analysis that follows and we give explicitly the expressions for all the form bilinears of the spinor (1.1). In appendix C, we give the linear system organized in G 2 representations. In appendices D and E, we present the solution of the linear system for generic as well as for special G 2 ⋉ R 8 backgrounds, respectively.
2 Solution of the Killing spinor equations

Killing spinor equations
The KSEs of (massive) IIA supergravity are the vanishing conditions of the supersymmetry variations of the fermions of the theory [10][11][12][13][14] evaluated at the locus where all fermions vanish. The conventions for the fields that we shall use, including the field equations and Bianchi identities, are as those in [4] which closely follow those of [14]. For completeness we state the KSEs of the theory, which are the vanishing conditions of where ∇ is the spin connection, H is the NS-NS 3-form field strength, S, F, G are the RR k-form field strengths, k = 0, 2, 4, and Φ is the dilaton. Note that the RR form field strengths in the KSEs have been rescaled with the exponential of the dilaton. The spinor ǫ is in the Majorana representation of Spin(9, 1), and ǫ is from now on taken to be commuting. The first KSE in (2.1) arises from the supersymmetry variation of the gravitino of the theory and is a parallel transport equation, while the second condition arises from the supersymmetry variation of the dilatino and is an algebraic equation on ǫ. In what follows, we shall seek solutions to the conditions Dǫ = Aǫ = 0 without making simplifying assumptions regarding the fields, the Killing spinor or the geometry of spacetime. For spinors, we use the same conventions as those employed in type IIB supergravity in the context of spinorial geometry [15], e.g. we choose Γ 11 = −Γ 01···9 .
2.2 Solution of the KSEs for the G 2 ⋉ R 8 backgrounds

Linear system and geometry
Applying spinorial geometry to the KSEs of (massive) IIA supergravity (2.1) for the spinor (1.1) turns these equations into a linear system with variables given by the components of the fluxes. This linear system is originally expressed in SU(3) representations and it is rather involved. This is because the expression for the Killing spinor (1.1) is manifestly SU(3) invariant. However, after some extensive computation the linear system can be recast into G 2 representations and this is given in appendix C. The equations of the JHEP06(2016)045 linear system depend on the fundamental G 2 forms ϕ and ⋆ϕ. As will become apparent below this is required so that, after a decomposition in G 2 representations, the equations of the linear system depend on the appropriate components of the fluxes and geometry.
To elucidate the notation and also give some preliminary description of the geometry of spacetime, note that all supersymmetric backgrounds which admit a Killing spinor with isotropy group H ⋉ R m , where H is a compact group, admit a no-where vanishing null 1-form e − for which its associated vector field K = g −1 e − is Killing. Such a 1-form splits the tangent space of the spacetime M as where I is the trivial real line bundle. To understand Ker e − , we choose a vector W such that e − (W ) = 1 and define the 1-form e + (Y ) = g(W, Y ). Clearly e + is not uniquely defined but all considerations are independent of the choice of e + . The metric g in such a case can be decomposed as Then Ker e − is spanned by K and all vectors Z which are perpendicular to both K and W , i.e. g(Z, K) = g(Z, W ) = 0. To decompose the flux form field strengths, one considers In such a case Ker K is spanned by e − and the 1-forms e I which are orthogonal to both e − and e + . The metric can then be written as Furthermore, a k-form flux can be decomposed as where (k), (k − 1) and (k − 2) denote the degree of the form in the directions orthogonal to both e + and e − . In the G 2 ⋉ R 8 case that we are investigating, there is an additional distinct 1-form e 1 that arises. This is due to the choice of the representative (1.1) of the Killing spinor. On the other hand, if one assumes that the spacetime globally admits a G 2 ⋉ R 8 invariant Killing spinor, the structure group of the spacetime reduces to a subgroup of G 2 so topologically the tangent space splits as T M = I 3 ⊕ E. There are thus three no-where vanishing vector fields on the spacetime which can be chosen such that their associated 1-forms are e + , e − , e 1 . In either case, the metric and k-form fluxes can be decomposed as where e i span the seven directions orthogonal to e + , e − , e 1 in E, and where a, b, c = +, −, 1 and the superscript in brackets (n) denotes the degree of the form along E. The components of the fluxes, as well as those of the spin connection Ω, that appear in the linear system in appendix B are defined according to the above decomposition.

Solution for the fluxes
The components of the fluxes along E can be further decomposed in G 2 representations. As G 2 ⊂ Spin (7) acts with the fundamental 7-dimensional representation on the typical fibre of E, the 2-forms decompose as 7 ⊕ 14, and the 3-and 4-forms decompose as 1 ⊕ 7 ⊕ 27. Using these decompositions, the 4-form, 3-form and 2-form fluxes can be written as respectively, where we have suppressed the degree of the forms along E.
The solution of the linear system as described in appendix D expresses some of the above components of the fluxes in terms of geometry as well as in terms of some other components of the fluxes which are not restricted by the KSEs. To relate the above decomposition of the fluxes in G 2 representations with the expressions in appendix D observe that the decomposition of 2-forms, 3-forms and 4-forms along E can be written as follows. For the 2-forms, we have where χ 14 ij ϕ ij k = 0 and For the 3-forms, we obtain where 15) and the notation (··) o , which we adopt from now on, denotes the symmetric traceless part of the two indices in the round brackets. Similarly for the 4-forms, we have where

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Using these definitions the solution of the linear system can be read off from appendix D.
There are many ways to arrange the solution of the linear system in appendix C. The arrangement that we follow is to express the components of the forms with higher degree, like G and H, in terms of the components of the forms of lower degree and the geometry. In particular for the G fluxes we have the following. The  Finally, the condition (D.25) can either be seen as a condition that restricts the dilaton or as a condition on the geometry of the spacetime. The latter case will be investigated below. Furthermore the rotation of K is restricted. For this observe that the sub-bundle Ker K ⊂ T * M further splits as Ker K = I ⊕ L, where I is spanned by e 1 . In addition, Λ 2 (L) decomposes in G 2 representations as Λ 2 (L) = Λ ′ 7 ⊕ Λ 7 ⊕ Λ 14 which have typical fibres R 7 , R 7 and g 2 , respectively. The rotation de − is a section of Λ ′ 7 ⊕ I ⊕ Λ 14 (L). In JHEP06(2016)045

Geometry of
Therefore the solution satisfies a g 2 instanton condition with an additional null component. It remains to investigate the remaining two conditions (D.22) and (D.25). Both these conditions are scalar conditions. The former condition puts a restriction on the G 2 structure of the spacetime. In fact, it restricts the singlet part of dϕ. In particular, (D.22) can be rewritten as The latter condition can also be interpreted as a restriction on the dilaton Φ. As a geometric condition it can be rewritten as Again it restricts the singlet class in the decomposition of ∇ i ϕ 1jk in terms of G 2 representations.
3 Special case (f = g) A special case arises whenever the 1-form bilinear κ(ǫ,ǫ) vanishes, see appendix B. As this bilinear by construction is covariant, such a condition can be implemented covariantly over the whole spacetime. In the gauge that we are working this implies that f 2 = g 2 and so f = ±g. In such case, the solution of the linear system simplifies dramatically. We shall take f = g = 1/ √ 2. The other case can be treated symmetrically.

Fluxes
As the expression of the fluxes in terms of the geometry is relatively simple, we shall present the fluxes in a closed form. In particular, we have that the 4-form flux is and the 2-form flux is Notice that the KSEs do not restrict all components of the fluxes in terms of the geometry. In fact, there are several components that remain unrestricted. Of course, these are determined by the field equations and Bianchi identities of the theory.

Geometry
The restrictions on the geometry of the backgrounds imposed by supersymmetry are as those of the general case described in (1.2). Moreover as f and g are constant, there is a simplification of the additional condition (2.19) which can now be written as in (1.4) which is the vanishing of the 1 representation of dϕ. It is well-known that this is one of the Gray-Hervella type of classes for G 2 structures [8,9]. Therefore the G 2 structure of the spacetime is of restricted type. The condition (2.20) also simplifies and in the special case reads as Again this condition can either be thought as a condition on the geometry or as an equation which determines the dilaton in terms of the geometry.

Concluding remarks
We have shown that the existence of a G 2 ⋉ R 8 Killing spinor on (massive) IIA backgrounds imposes rather weak conditions on the geometry. In particular, the backgrounds are required to admit a null Killing vector which leaves the Killing spinor invariant, and the rotation of the Killing vector is required to satisfy a G 2 instanton condition with an additional non-vanishing null component. There are two additional scalar conditions given in (2.19) and (2.20) which thus do not impose strong conditions on the geometry. It is remarkable that these conditions on the geometry are similar to the ones we have found JHEP06(2016)045 for (massive) IIA backgrounds admitting SU(4) invariant Killing spinors [5]. In particular, SU(4) backgrounds admit a time-like Killing vector field which also leaves the Killing spinor invariant. The SU(4) backgrounds also admit another vector field which commutes with the Killing vector field, and impose some additional scalar conditions on the geometry. However the geometry of IIA backgrounds admitting either Spin (7) or Spin(7) ⋉ R 8 invariant Killing spinors satisfy stronger conditions [4]. This is because apart from the existence of appropriate Killing vector fields which leaves the Killing spinor invariant an additional condition, which transforms as a spinor under Spin (7), is required. Another characteristic of Spin (7), SU(4) and G 2 ⋉ R 8 backgrounds is the existence of special cases for which the solution of the KSEs simplify dramatically. All three special cases arise as a requirement for the vanishing of a certain spinor bilinear. As all these transform covariantly on the spacetime, these vanishing conditions can be imposed consistently over the whole spacetime. The existence of such special spinors is reminiscent of the existence of pure spinors in Euclidean signature spaces. Pure spinors are complex and can also be defined as those for which a certain vector bilinear vanishes. As pure spinors are related to complex structures, there may be a similar geometric interpretation for the Killing spinors that occur in all three special cases; though of course in IIA the spinors are real and it is not in all cases a vector bilinear that is required to vanish.
As we have already mentioned in the introduction, since the rank of the spinor bundle of IIA backgrounds is much larger than the dimension of the spacetime, the mere existence of a no-where vanishing spinor does not imply the reduction of the structure group of the spin bundle. As a result G-structures are not useful for the global description of the geometry of spacetime. This is also the case even when one adapts a generalized geometry approach to characterize the backgrounds in terms of the isotropy groups of the components of the Killing spinors in the two different sectors. In the context of IIA theory, this is to characterize the backgrounds in terms of the isotropy groups of chiral and anti-chiral components of the Killing spinors. In the case of one supersymmetry, these are Spin(7) ⋉ R 8 × Spin(9, 1) for a Spin(7) ⋉ R 8 -invariant Killing spinor, Spin(7) ⋉ R 8 × Spin(7) ⋉ R * 8 for a Spin(7)-invariant Killing spinor, Spin(7) ⋉ R 8 × Spin(7) ⋉ R * 8 for an SU(4)-invariant Killing spinor, and Spin(7) ⋉ R 8 × Spin(7) ⋉ R 8 for a G 2 ⋉ R 8 -invariant Killing spinor, where R * 8 denotes the other lightcone direction compared to that of R 8 . However, such a characterization may work well in the special cases where the two chiral components never vanish, like that of the common sector, but for generic IIA backgrounds this may not always be the case. So such a characterization is not useful in general type II theories. Spinorial geometry [6], on the other hand, can be adapted to treat all cases simultaneously. For this it suffices to choose a Killing spinor representative which includes all the Killing spinors with the four different isotropy groups as special cases. There are examples already of such a treatment. The first example is the IIA Spin(7) backgrounds which include those with Spin(7) ⋉ R 8 invariant Killing spinors as a special case. Another example is the Killing spinors of G 2 ⋉ R 8 backgrounds which include the Killing spinors of the Spin(7) ⋉ R 8 backgrounds as special cases whenever f or g vanishes. In the general case, the construction of the linear system will be straightforward. However, it will be more involved than the ones we have considered so far for two reasons. First, it will depend on JHEP06(2016)045 many more functions like f and g in (1.1), and second, as the manifest symmetry of the Killing spinor representative will be much smaller compared to the backgrounds we have investigated here, the linear system will decompose into many more equations. As a result, the solution will be more difficult to find, but since we have a computer implementation of the analysis this is not a problem. In any case, spinorial geometry provides a method to solve the KSEs of backgrounds for which the isotropy group of the Killing spinor changes from patch to patch, as has already been demonstrated in the examples mentioned above. As the change of isotropy group of the Killing spinor is expected to be a widespread phenomenon, for example all spacetimes which exhibit a Killing horizon with respect to the Killing vector bilinear belong to this category, it will be fruitful to pursue this in the future.

A Conventions and useful formulae
Our IIA supergravity conventions including the form of the KSEs, Bianchi identities and field equations are those of [4], which are similar to those of [14]. Our spinor conventions can be found in [15].

A.1 Spinors
The Dirac spinors of spin(9, 1) can be identified with the space of forms Λ * (C 5 ). Equipping C 5 with a Hermitian basis e 1 , . . . , e 5 , the gamma matrices act as Γ 0 = −e 5 ∧ + e 5 , Γ 5 = e 5 ∧ + e 5 , Γ r = e r ∧ + e r , Γ r+5 = i(e r ∧ − e r ) , (A.1) for r = 1, 2, 3, 4, where ∧ and are the wedge product and the inner-derivation operators on the space of forms, respectively. In this realization of the spinor representations, the spinors can be written as multi-forms. The KSEs, Bianchi identities and field equations of (massive) IIA supergravity are invariant under local Spin(9, 1) transformations. In spinorial geometry [6], these can be used to choose a representative for the Killing spinor (1.1). Notice that this representative in the present case is a linear combination of the multi-forms 1 + e 1234 and e 1 + e 234 , where in e 1234 and e 234 the wedge product symbol between the Hermitian basis elements has been suppressed. Then a computation reveals that the isotropy subgroup of both 1 + e 1234 and e 1 + e 234 in spin(9, 1) is G 2 ⋉ R 8 . To see this it suffices to find the generators of spin(9, 1) that annihilate the two spinors above using the realization for the gamma matrices in (A.1).
In the context of spinorial geometry [6], the choice of a representative for the Killing spinor introduces a class of compatible frames on the spacetime. In this particular case, the choice of (1.1) for the Killing spinor introduces a frame basis (e 0 , e 5 , e 1 , e i ), where i = 2, 3, 4, 6, 7, 8, 9, adapted to the choice of gamma matrices in (A.1). Equivalently, one can also introduce a lightcone basis (e − , e + , e 1 , e i ), where e ± = 2 − 1 2 (±e 0 + e 5 ), which is JHEP06(2016)045 used throughout as it is more useful in the description of the geometric data. Note for example that Γ − = e − M Γ M = √ 2e 5 annihilates the Killing spinor (1.1). Furthermore, observe that under a boost in the 5th direction, which is a local symmetry of the theory, the functions f and g in (1.1) transform as f → e h f and g → e h g, where h is a function on the spacetime generating the boost. This symmetry can be used for choosing the gauge f 2 + g 2 = 1 that we use. In this gauge, the frame e − can also be identified, up to a sign, with a 1-form Killing spinor bi-linear, see appendix B.
A.2 G 2 fundamental forms The linear system that arises from the KSEs in the context of spinorial geometry is initially expressed in terms of SU(3) representations which is the manifest symmetry of the Killing spinor (1.1). However, the linear system can be re-expressed in terms of G 2 representations, which is the isotropy group of the Killing spinor (1.1). This requires the use of the fundamental G 2 3-form and its 4-form dual where ω = −(e 2 ∧ e 7 + e 3 ∧ e 8 + e 4 ∧ e 9 ) , χ = (e 2 + ie 7 ) ∧ (e 3 + ie 8 ) ∧ (e 4 + ie 9 ) , and the Hodge operator is taken with respect to the volume form e 2 ∧e 3 ∧e 4 ∧e 6 ∧e 7 ∧e 8 ∧e 9 .
As the initial formulation is in terms of SU(3) representations, we need expressions for the fundamental forms of G 2 in terms of the fundamental forms of SU(3).
In the Hermitian basis, which arises in the initial construction of the linear system. We also have and where 1 and1 are holomorphic and anti-holomorphic indices, respectively. Using these formulae, one can easily find the various contractions of ϕ and ⋆ϕ as 14) which are useful in many of the computations we have performed, where This summarizes G 2 fundamental form identities.

A.3 Covariant derivatives of fundamental forms
In the linear system, various components of the spin connection appear. Because of this it seems that the associated relations are not covariant. However, this is not the case provided that the patching conditions of the spacetime are compatible with the underlying G 2 structure. This is enforced by the observation that all components of the spin connection that appear in the linear system can be re-expressed as appropriate covariant derivatives on the fundamental forms ϕ, ⋆ϕ, e + , e 1 and e − . In particular, we have where A, B, C are spacetime frame indices. These give rise to the identities where a, b = −, +, 1, i.e. A = {a, i}, where i is a seven-dimensional index labelling the G 2 -directions. We use the formulae above to express the conditions on the geometry in terms of the fundamental forms.

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B The spinor bilinears of G 2 ⋉ R 8 spinors The IIA spinors are Majorana, so for the computation of the bilinears one can use either the Majorana or Dirac inner products. The conventions for these can be found in [15]. In IIA supergravity, apart from the Killing spinor ǫ in (1.1), one can define another globally defined spinorǫ = Γ 11 ǫ which is not necessarily Killing. The form bilinears of ǫ andǫ are two 1-forms and two 5-forms where ϕ is the invariant G 2 3-form defined in the previous appendix and we have normalised the Killing spinor with an additional factor of 1/ √ 2. It is convenient in many computations to take the gauge f 2 + g 2 = 1. C The linear system for the G 2 ⋉ R 8 invariant spinor C.1 Dilatino Killing spinor equation The linear system that arises from the KSEs in the context of spinorial geometry can be organized in the scalar, vector (or equivalently 7), 2-form, symmetric traceless (or equivalently 27) G 2 representations. In particular, the conditions that arise from the dilatino KSE are as follows.

C.1.1 Conditions in the scalar representation
The conditions that transform as scalars are As we shall see later the solution of these conditions simplifies in the gauge f 2 + g 2 = 1.

C.1.2 Conditions in the vector representation
The conditions that transform as vectors are f H+j 1 j 2 ϕi j 1 j 2 = 0, (C.5) Note that the dilatino KSE gives rise to only scalar and vector conditions.

C.2 Gravitino Killing spinor equation C.2.1 Conditions in the symmetric traceless representation
The conditions that lie in the 27 representation are As we shall show below these conditions impose restrictions on both the geometry and fluxes of the theory.

C.2.2 Conditions in the 2-form representation
The conditions that arise from the gravitino KSE which are organized in the 2-form representation are (C.16)

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The above conditions can be decomposed further into the 7 and 14 G 2 representations. In particular the 7 component of (C. 15) and (C.16) can be expressed as They will used later together with other conditions in the vector representation to solve the linear system for the fluxes.

C.2.3 Conditions in the vector representation
The most involved set of conditions that arise in the linear system are those that lie in the 7 representation. These are as follows f Ω−,+i = 0, (C.32) The solution of these conditions, together with the vector representation conditions that we derived from the 2-form representation above and those that we have found from the dilatino KSE, gives a large number of relations between the components of the fluxes as well as conditions on the geometry of spacetime.

C.2.4 Conditions in the scalar representation
Finally, the conditions that arise in the scalar representation of G 2 are Ω +,+1 = 0, (C.34) JHEP06(2016)045 The solution of these conditions, as well as all the others we have derived from the dilatino and gravitino KSEs, will be given in the next appendix.
on the geometry, and the conditions on the fluxes. In particular, observe that most of these fluxes vanish.

D.2 Solution of the rest of the scalar conditions
The next task is to solve all the remaining scalar conditions of the linear system that arises from the gravitino and dilatino KSEs in the context of spinorial geometry. In particular combining (C.37) and (C.38), we find Then set C ′ = C + (f 2 − g 2 )D, where C ′ ≡ 1 3 G 1ijk ϕ ijk + 4f gH −+1 − 4f gΩ i,jk ϕ ijk − 6F −+ + 8(f 2 − g 2 )S = 0 , (D.8)

D.4 Solution of the rest of 2-form conditions
It remains to investigate the 14 representation content of the (C. 15) and (C.16) conditions as the 7 representation has already been taken into account. In particular, one finds that