Consistent $S^3$ reductions of six-dimensional supergravity

We work out the consistent AdS$_3\times S^3$ truncations of the bosonic sectors of both the six-dimensional ${\cal N}=(1,1)$ and ${\cal N}=(2,0)$ supergravity theories. They result in inequivalent three-dimensional half-maximal ${\rm SO}(4)$ gauged supergravities describing 32 propagating bosonic degrees of freedom apart from the non-propagating supergravity multiplet. We present the full non-linear Kaluza-Klein reduction formulas and illustrate them by explicitly uplifting a number of AdS$_3$ vacua.


Introduction
Consistent sphere truncations have a long history in supergravity. Within maximal supergravity, this goes back to the seminal work of [1] on the consistent truncation of eleven-dimensional supergravity on AdS 4 × S 7 to the lowest Kaluza-Klein multiplet giving rise to four-dimensional SO(8) gauged supergravity. An analogous result for AdS 7 × S 4 was established in [2], while the proof of the consistent truncation of IIB supergravity on AdS 5 × S 5 was completed only recently [3]. Consistent truncations have led to a better comprehension of the structures of the theories of concern and the dualities they enjoy. Notably, these are not truncations in an effective field theory sense, with the massive Kaluza-Klein towers integrated out, yet every solution of the lower-dimensional theory lifts to a solution of the higher-dimensional theory. They are of particular importance in holographic applications, ensuring the validity of lower-dimensional supergravity computations, such as holographic correlators and renormalization group (RG) flows [4].
This work deals with consistent sphere compactifications in the context of AdS 3 × S 3 , one of the central examples in the AdS/CFT correspondence [5] in which supergravity techniques have been successfully employed [6][7][8][9][10][11] in order to unravel the structure of the dual two-dimensional conformal field theories. Generic consistent S 3 truncations in (super)gravity have been discussed in [12][13][14], where the full non-linear Kaluza-Klein Ansätze were constructed for a higherdimensional theory that comprises the field content of the bosonic string. The resulting lowerdimensional theories are SO(4) gauged (super)gravities carrying gauge fields, a 2-form, and scalar fields whose potential do not admit any stationary points. In the particular case of AdS 3 × S 3 , the higher-dimensional theory is D = 6, N = (1, 0) supergravity coupled to a single tensor multiplet that carries an anti-selfdual 2-form. In contrast to the higher-dimensional examples, the 2-forms in the resulting three-dimensional theory are auxiliary and can be integrated out, giving rise to an additional contribution to the scalar potential. This amended potential turns out to support a stable supersymmetric AdS 3 vacuum [15], corresponding to the supersymmetric AdS 3 × S 3 solution of the D = 6 theory. The non-linear Kaluza-Klein Ansätze can be confirmed by direct computation.
The paper is organized as follows. In section 2, we introduce the relevant three-dimensional supergravities, their gauge structure and scalar potentials. We give an explicit parametrization of their scalar target space SO(8, 4)/ SO(8) × SO(4) and determine the full set of stationary points of their scalar potentials. In section 3, we review the framework of SO (8,4) ExFT. In particular, we discuss the two inequivalent solutions of its section constraint and establish the full dictionary of the ExFT fields into the six-dimensional fields of N = (1, 1) and N = (2, 0) supergravity, respectively. In sections 4 and 5, we use the explicit Scherk-Schwarz twist matrix U together with the ExFT-supergravity dictionary to work out the full non-linear Kaluza-Klein Ansätze for all six-dimensional fields, defining the consistent truncation. As an illustration and a consistency check, we use these Ansätze in section 6 in order to give the explicit uplift of some of the three-dimensional AdS 3 vacua into full solutions of D = 6 supergravity. We close with some comments in section 7.

The three-dimensional supergravity
In this section, we collect the basic formulas of the relevant three-dimensional supergravities. In particular, we give an explicit parametrization of their scalar target space, which allows us to determine the full set of stationary points of the scalar potentials.

3D gauged supergravity
Three-dimensional gauged supergravity with N = 8 (half-maximal) supersymmetry has been constructed in [22,23]. The theory is based on the coset space with all couplings completely specified by the choice of a constant symmetric embedding tensor ΘKL ,MN of the form with antisymmetric θKLMN = θ [KLMN ] , symmetric θMN = θ (MN ) and the SO(8, 4) invariant tensor ηMN . IndicesM ,N , . . . label the vector representation of G = SO (8,4), and are raised and lowered with ηMN . The embedding tensor encodes the minimal coupling of vector fields to scalars according to with the symmetric matrix MMN parametrizing the coset space (2.1). By TMN we denote the generators of g = Lie G acting by left multiplication with the algebra The number of vector fields involved in the connection (2.3) is equal to the rank of ΘKL ,MN (taken as a dim G × dim G matrix). The complete bosonic Lagrangian of the three-dimensional theory is given as a gravity coupled Chern-Simons gauged G/H coset space σ-model with three-dimensional metric g µν and e ≡ |det g µν | . The Chern-Simons term is explicitly given by in terms of the embedding tensor (2.2), with the SO(8, 4) structure constants fMN ,PQRS from (2.4). The form of the scalar potential V is determined by the embedding tensor and may be written in the form [24] (where we have corrected a typo in the second line) From the general expression of the scalar potential, we have omitted the term carrying a totally antisymmetric MKLMNPQRS which drops out upon restriction to embedding tensors satisfying the additional constraint As pointed out in [21], consistent truncations obtained by generalized Scherk-Schwarz reduction necessarily lead to three-dimensional theories satisfying (2.8), and we will in the following restrict to such theories. For the fermionic completion of (2.5) and its full supersymmetry transformations we refer to [22,23]. For the following, it will be convenient to choose a specific basis upon breaking with A = 1, . . . , 4 and α = 1, . . . , 4 labelling the GL(4) and the SO(4) vector representation, respectively. In this basis, the GL(4) is embedded into an SO (4,4), such that the SO (8,4) tensor is of the form Specifically, we will be interested in the theories described by the two embedding tensors with the totally antisymmetric ε ABCE , a free constant α. These theories capture the S 3 reductions of N = (1, 1) and N = (2, 0) supergravity, respectively. In particular, the embedding tensors induce the gauge connections in the second case. Both embedding tensors induce a gauge group of non-semisimple type with the abelian generators T AB of T 6 transforming in the adjoint representation of SO(4) . Chern-Simons gauge theories with gauge group of type (2.14) and the T 6 generators realized as shift symmetries on scalar fields can be rewritten as SO (4)

Parametrization of the SO(8, 4)/ SO(8) × SO(4) scalar coset
In order to study the structure of the scalar potential (2.7), it turns out to be useful to adopt particular parametrizations of the scalar matrix MMN . To this end, we decompose the SO(8, 4) generators according to (2.9), such that a coset element V ∈ SO(8, 4)/ SO(8) × SO(4) can be parametrized in triangular gauge as with nilpotent generators T AB = T [AB] and a GL(4) matrix V GL (4) . Modula an SO(4) gauge freedom, this matrix carries the 32 physical scalar degrees of freedom. In the following, we will make use of the fact that the gauge groups we are studying include shift symmetries acting on the scalars φ AB , c.f. (2.12), which we may use to adopt a gauge in which φ AB → 0. As a result, the gauge group (2.14) reduces to a standard SO(4) . Explicitly, we choose a representation such that Evaluating the scalar kinetic term from (2.5) in this parametrization yields and SO(4) covariant derivatives D µ . The first term in (2.18) represents a GL(4)/SO(4) σ-model. Let us finally evaluate the scalar potential for the two choices of embedding tensor (2.11). For the embedding tensor (A), describing the N = (1, 1) reduction on S 3 , the potential (2.7) depends exclusively on the block M AB . In the parametrization (2.17), the potential is thus independent of the scalars φ Aα . Explicitly, it takes the form where we have defined with detm AB = 1 . This precisely agrees with the result of [15] as required by consistency since the additional scalar fields φ Aα do not show up in the potential. Note that rescaling ϕ → ϕ − log |α| turns the constant α into a global scaling factor in front of the potential, which is thus irrelevant for the existence of stationary points. Depending on the sign of α there are however two different fermionic completions of the theory. In contrast, for the embedding tensor (B) from (2.11), describing the N = (2, 0) reduction on S 3 , the potential after some computation takes the form where again we used the parametrization (2.21). We note that for φ Aα = 0, this expression coincides with the potential (2.20) upon flipping This is consistent with the fact that upon setting the φ Aα fields to zero, both the N = (1, 1) and the N = (2, 0) theories reduce to the same N = (1, 0) theory in six dimensions, which gives rise to the potential computed in [15]. Again, the constant α can be absorbed by shifting ϕ together with a rescaling of φ Aα . However, the presence of a term linear in α implies that there are two inequivalent theories depending on the sign of α which cannot be absorbed into a field redefinition. In the following, we will adopt the normalization |α| = 1 .

Extrema of the scalar potential
In this section, we derive the full set of extremal points of the scalar potentials (2.20) and (2.22). Since (2.20) sits within (2.22) as a truncation φ Aα = 0, it will be sufficient to analyze the extremal points of the latter. Below we will then uplift some of these extremal points to solutions of the six-dimensional supergravities. Variation of (2.22) with respect to the scalar field ϕ yields the condition Next, let us consider the variation with respect to the φ Aα , such that δ Σ (φφ) AB = Σ Aα φ Bα + Σ Bα φ Aα . Variation of the potential yields such that extremization leads to the eigenvector equation Finally, variation with respect to the SL(4) scalars according to Upon reducing the last term by means of (2.26), this equation can be solved for (φφ) AB as with χ = 2 α − 1 2 (φφ) DD . Plugging this expression back into the eigenvector equation (2.26) eventually implies The conditions for stationary points thus boil down to solving equations (2.24) and (2.29). The value of the potential at an extremal point is computed by evaluating (2.22) using (2.24) and (2.26) which corresponds to a three-dimensional AdS length withg µν denoting the AdS 3 metric. Let us first consider the sector φ Aα = 0, which is a consistent truncation of the potential (2.22) and contains the stationary points common to (2.20) and (2.22). In this case, equation (2.26) is trivially satisfied. Solutions of the remaining equations (2.24), (2.27) are most conveniently found in a basis in whichM AB is diagonal. Inspection reveals a one-parameter family of solutions given by (2.32) The existence of this flat direction in the scalar potential has already been noted in [26]. The potential for these families remains fixed at V (B),0 = −2, and the scalar spectrum is given by for the different potentials. These spectra are stable (in the Breitenlohner-Freedman sense The vector spectrum is given by reflecting the unbroken SO(2) × SO(2) ⊂ SO(4) . Finally, the gravitino spectrum is given by showing that only for α = −1, the vacuum at η = 0 is supersymmetric, preserving N = (4,4) supersymmetry. This corresponds to the six-dimensional supersymmetric background AdS 3 ×S 3 . The α = +1 solution is not supersymmetric, but may correspond to a supersymmetric solution in an N = (1, 0) theory coupled to tensor multiplets. The potential (2.22) allows for additional stationary points with φ Aα = 0 . In this case, the remaining equations (2.24), (2.29) again are most conveniently solved in a basis in whichm AB is diagonal, where we find 4 discrete solutions. They all necessitate positive α = +1 with the potential taking the values .
(2.38) All these stationary points fully break supersymmetry and SO(4) gauge symmetry, and they all contain unstable scalars with masses below the Breitenlohner-Freedman bound m 2 ℓ 2 = −1. For later checks, let us only note the location of solution (i) with the scalar mass spectrum given by

SO(8, 4) exceptional field theory
In this section, we review the structure of SO (8,4) ExFT, constructed in [21], to which we refer for details. This theory provides the manifestly duality covariant formulation of the 6D supergravity theories relevant for our consistent truncations. We discuss the inequivalent solution to its section constraints and establish the dictionary of the ExFT fields to the 6D fields of N = (1, 1) and N = (2, 0) supergravity theories, respectively.

Lagrangian
Similar to the three-dimensional supergravities reviewed in section 2, SO (8,4) ExFT is based on the coset space (2.1) which we parametrize by a symmetric positive definite matrix M M N . In contrast to the matrix of (2.17), this matrix depends not only on three external coordinates x µ , but in addition on (dim SO(8, 4)) coordinates Y M N with the latter dependence strongly constrained by the section conditions which restrict the fields to live on sections of dimension three (at most). Depending on the choice of these sections, the theory describes the 6D N = (1, 1) or N = (2, 0) supergravity, respectively. The theory is invariant under generalized internal diffeomorphisms, acting as on the scalar matrix. Here, the gauge parameters Σ M N are subject to algebraic constraints analogous to (3.1), i.e.
as well as compatibility with the partial derivatives as The full Lagrangian is given by Finally, the last term in (3.6) carries only internal derivatives ∂ M N and is given by Depending on the solution of the section constraints (3.1), the action (3.6) describes 6D N = (1, 1) or N = (2, 0) supergravity. In the next two subsections, we review the two inequivalent solutions to the section constraints and the associated dictionaries of the ExFT fields into the 6D supergravity fields.  11) where subscripts refer to the sum of the GL(1) ⊂ GL(3) charge and the SO(1, 1) charge, defining the grading associated to the higher-dimensional origin of these fields. Here i = 1, 2, 3 and α = 1, . . . , 4. The invariant tensor η M N decomposes accordingly (3.12) The N = (1, 1) solution to the section constraints (3.1) is given by decomposing coordinates Y M N according to (3.11) and restricting the internal coordinate dependence of all fields to the coordinates Y 0i , such that the only non-vanishing internal derivatives are providing a solution to (3.1). Breaking the ExFT fields according to (3.11), then matches the field content of the 6D N = (1, 1) supergravity which, in addition to the metric and the dilaton, contains 4 vector fields and a (non-chiral) 2-form gauge field. Specifically, the ExFT vector fields transform in the adjoint representation of SO (8,4). Under (3.11), they decompose into +1 : . . . , (3.14) allowing to identify the higher-dimensional origin of the various components. The fields of positive grading do not enter the action (3.6). Similarly, one decomposes the scalar fields, parametrizing the coset SO(8, 4) (SO(8) × SO(4)) into ⊂ 6d dual 3-form +2 : φ i 0 , φ ij ⊂ 6d 2-form and its dual +1 : φ iα ⊂ 6d vectors 0 : g ij , ϕ ⊂ 6d metric and dilaton .
where we have redefined the gauge parameters as with the totally antisymmetric ε ijk . Here, L λ denotes the standard Lie derivative along the vector field λ k . Identifying the higher-dimensional origin of the gauge parameters among internal 6D diffeomorphisms and gauge transformations according to the identification of the vector fields (3.14) then allows to read off the dictionary between the components of M M N and the internal components of the 6D fields The dictionary is such that the generalized diffeomorphisms (3.2) reproduce the gauge transformations of the 6D vector fields A i α , 2-form B ij and its dualB ij . Finally, using the dictionary (3.18), we may also consider from which we infer the identification with the scalars a ijk α from the dual 3-forms in six dimensions. These transform as under 6D gauge transformations. Later on, we will also decompose a −→ {0, α} . The N = (2, 0) solution to the section constraints (3.1) is given by decomposing coordinates Y M N according to (3.23) and restricting the internal coordinate dependence of all fields to the coordinates Y ij , such that the only non-vanishing internal derivatives are

Consider the decomposition of SO(8, 4) under its subgroup GL(3) × SO(1, 5) such that the fundamental SO(8, 4) vector decomposes as
providing a solution to (3.1). Breaking the ExFT fields according to (3.23) then matches the field content of the 6D N = (2, 0) supergravity coupled to a tensor multiplet, which contains 5 selfdual and 1 anti-selfdual 2-form gauge fields, together with 5 scalar fields parametrizing the coset space SO(1, 5)/SO(5) . Specifically, the ExFT vector fields transform in the adjoint representation of SO (8,4). Under (3.23), they decompose into with the gauge parameter relabelled as These let us infer the dictionary with g ≡ det g ij , and the components B ijā transform under tensor gauge transformations as

Generalized Scherk-Schwarz reduction
Consistent truncations of SO (8,4) ExFT can be defined by a generalized Scherk-Schwarz compactification ansatz [17,18], in which the dependence of the ExFT fields on the internal coordinates is carried by an SO(8, 4) twist matrix U MN and a scalar factor ρ. Specifically, the ExFT fields take the factorized form [21] 3.32) in terms of the x-dependent fields of 3D gauged supergravity reviewed in section 2 above. The embedding tensor (2.2) of the 3D theory is given in terms of the twist matrix as and the truncation is consistent if all three objects in (3.33) are actually Y -independent. Using the twist matrices from [21] we will, in the following, use the generalized Scherk-Schwarz ansatz in order to derive the explicit reduction formulas for the 6D consistent truncations.

N = (1, 1) uplift formulas
In this and the following section, we will review from [21] the twist matrices inducing the embedding tensors (2.11). Combining them with the ansatz (3.32) and the supergravity dictionaries worked out in sections 3.2, 3.3 above, we deduce the six-dimensional N = (1, 1) and N = (2, 0) reduction formulas.

Twist matrix
The SO(8, 4) twist matrix U MM describing the consistent S 3 truncation of 6D N = (1, 1) supergravity has been constructed in [21]. Let us recall that the coordinates y i relevant for 6D N = (1, 1) supergravity have been identified among the Y M N via (3.13). The associated twist matrix is given in terms of the elementary S 3 sphere harmonics Y A (satisfying Y A Y A = 1), the round S 3 metricg ij = ∂ i Y A ∂ j Y A (with determinantg), and the vector fieldζ i defined bẙ ∇ iζ i = 1. Byω ijk ≡g 1/2 ε ijk , we denote the associated volume form. We refer to appendix A for further identities among these objects. After some rewriting, the twist matrix of [21] takes the explicit form in a basis where the 'curved index' M is decomposed according to (3.11), and the 'flat index'M is decomposed in the basis (2.9), suitable for the fields of 3D supergravity. The free parameter α can (up to sign) be absorbed into a shift of the 6D dilaton.

Uplift formulas
According to the dictionary (3.18), the 6D dilaton is identified within the component M 00 of the ExFT scalar matrix, such that its reduction formula is obtained via (3.32) as where we have defined the warp factor Similarly, we identify the internal components of the 6D 2-form as giving rise to Further computation yields the 6D internal (inverse) metric Identifying the SO(4) Killing vectors K AB i =g ij ∂ j Y [A Y B] on the right hand side, this result reproduces the standard Kaluza-Klein ansatz for the internal metric [28]. Using sphere harmonics identities collected in appendix A, we may deduce the internal metric together with a compact expression for the warp factor (4.3) where we recall the definition (2.21) of the 3D scalar ϕ. The latter may be used to simplify the reduction formulas (4.2)-(4.7) as We thus obtain a compact form of the full 6D metric 10) and may also compute the internal component of the 3-form field strength We may compare these results to the reduction formulas found in [12,15] for the N = (1, 0) subsector and find precise agreement upon applying the dictionary The present construction extends these formulas to the full N = (1, 1) theory. The additional matter is made from N = (1, 0) vector multiplets, whose reduction formulas are extracted from (3.18) as which upon combination with (4.9) and after some computation reduces to the simple formula showing that in particular the internal field strengths vanish Similarly, we extract the reduction formula for the dual 2-formB ij upon combining (3.18) with all previously obtained reduction formulas, and find Finally, we may work out the reduction formula for the internal components of the 6D 3-form (dual to the 6D vector fields) as Formulas (4.14) and (4.17) show that in the case of 3D constant scalar solutions, all 6D vector field strengths vanish, such that the embedding of the N = (1, 0) theory into the N = (1, 1) theory remains rather trivial. This reflects the fact that the potential (2.20) does not carry the additional 3D scalar fields φ Aα and thus coincides with the potential of the truncation to the quarter-maximal theory of [12,15]. In contrast, for solutions with running scalars, such as 3D RG flows in the potential (2.20), these formulas describe non-trivial 6D gauge fields.

N = (2, 0) uplift formulas
In this section, we repeat the analysis for the reduction of the N = (2, 0) theory. As already reflected by the richer structure of the 3D potential (2.22), in this case the uplift formulas to six dimensions constitute a rather non-trivial extension of the formulas [12,15] for the quartermaximal truncation.

Twist matrix
The twist matrix describing the consistent truncation of 6D N = (2, 0) supergravity has been given in [21] in terms of the same geometrical data introduced in section 4.1 above. Let us recall that the coordinates y i relevant for 6D N = (2, 0) supergravity have been identified in (3.25) above. In a basis where the 'curved index' M is decomposed according to (3.23), and the 'flat index'M is decomposed in the basis (2.9), the associated twist matrix is given by Again, the free parameter α can (up to sign) be absorbed into a shift of the 6D dilaton.

Metric
Combining the embedding (3.31) of the internal metric g ij into the scalar matrix with the twist ansatz (3.32) and the twist matrix (5.1), we read off where we have defined The matrix m AB denotes the GL(4) matrix constituting a 4 × 4 block of the matrix MMN (2.17) parametrizing the 3D coset space (2.1), the matrix m AB is its inverse. Some algebraic manipulation (c.f. (4.6) above) yields the explicit form of the inverse metric Comparison to (4.6), (4.8), and (4.9) above shows precise agreement with the reduction formulas obtained for the N = (1, 1) theory upon redefinition (2.23) of the 3D fields.

2-forms
In the same way, we extract the reduction formulas for the 6D 2-forms via the dictionary (3.31).
With the explicit form of the twist matrix (5.1), after some computation and use of the explicit formulas (5.2), (5.4), this gives rise to the expressions for the SO(4) vector of 2-forms, and for the remaining two 2-forms. For later use, it will be interesting to explicitly compute the associated field strengths H ijkā = 3 ∂ [i B jk]ā : where we have defined the rescaled∆ ≡ e ϕ ∆ .

Scalars
Eventually, we can compute the 6D scalar fields from the last line of (3.31) upon subtracting the B 2 term using explicit expressions from (5.5), (5.6) above. The five 6D scalars sit in a coset space SO(1, 5)/SO(5) which we parametrize by a symmetric positive definite matrix Māb. Evaluation of (3.31) yields the various components of this matrix as for the 2 × 2 block in (0,0) directions and for the remaining components.

Uplift formulas for the 3D vector sector
Building on the dictionary (3.26), we may also give the uplift of the 3D vector fields. We recall from section 2.1, (in particular (2.12)) that the 3D Lagrangian carries 12 vectors fields: 6 A µ AB and the 6 antisymmetric combinations A µ A B − A µ B A . Moreover, in the 3D gauge we are using (in which scalars φ AB are set to zero), the vector fields A µ A B can be eliminated by means of their algebraic field equations in terms of scalar currents and the field strengths ⋆F AB . For the off-diagonal block of the 6D metric, we thus find in terms of the 3D vector fields from (2.13) and the SO(4) Killing vectors and where we have used the relation (A.5). This consistently reproduces the standard Kaluza-Klein ansatz for the vector fields [28], such that upon combination with the result of section 5.2.1, the full 6D metric takes the form with Similarly, we can work out the reduction formulas for the off-diagonal blocks of the 6D 2-forms, leading to Note that the vector fields A µ Aα do not appear in the Lagrangian (2.5), can be defined on-shell and subsequently be set to zero by a suitable (tensor) gauge transformation. The complete 6D 2-forms are then given by where the first two terms have been given in (5.5), (5.6) and (5.13), respectively, while the missing components B µνā are most conveniently obtained directly from the 6D tensor selfduality equations which allow to express their field strengths H µνρā in terms of the associated H ijkā , computed in (5.7).

Some explicit uplifts
In order to illustrate and check the non-linear uplift formulas obtained, we will now use them to uplift some of the AdS 3 solutions corresponding to the stationary points of the 3D scalar potential to full solutions of 6D supergravity.
6.2 One-parameter deformation of AdS 3 × S 3 As a first example, we give the 6D uplift of the non-supersymmetric but stable one-parameter family of AdS 3 solutions (2.32) located at m AB = diag e η , e η , e −η , e −η , φ Aα = 0 , The six-dimensional metric is then obtained from (5.11) as a warped product of AdS 3 and a deformed sphere S 3 ds 2 6 = ∆ −2 ds 2 AdS 3 + dθ 2 + e η ∆ 2 cos 2 θ dξ 2 1 + e −η ∆ 2 sin 2 θ dξ 2 2 , (6.6) with the two surviving U(1) isometries corresponding to rotations along ξ 1 and ξ 2 . The full 6D curvature scalar follows as The SO(1,5) scalars are computed from (5.8) as 8) and the components of the 3-form field strengths along the S 3 directions follow from (5.7) to be The remaining components of the 6D field strengths can then be determined by imposing the 6D self-duality equations (6.2), giving rise to and vanishing H α . The field strengths are given in terms of the volume formsω S 3 ,ω AdS of unitlength S 3 and AdS 3 , respectively. The Bianchi identities constitute a non-trivial consistency check of this result. Furthermore, it is straightforward to check that all 6D second order field equations (6.1) are indeed satisfied for α 2 = 1.

Uplift of an AdS 3 vacuum
As a second example, let us work out the 6D uplift of the stationary point (i) (2.38) of the potential (2.22). Although this solution is unstable as an AdS 3 vacuum, thus not of immediate interest, the fact that its uplift solves all 6D field equations constitutes a non-trivial consistency check to our uplift formulas. Recall that the location of this solution is specified by (2.39) with m ≡ 3/2. Using the explicit parametrization introduced earlier (6.4) for the sphere harmonics, one now finds a constant warp factor ∆ = m −3/4 . Then the six-dimensional metric is readily obtained as ds 2 6 = m 3/2 ds 2 AdS + m −1/2 ds 2 S 3 . (6.11) The Ricci tensor of this metric can be conveniently given as Rμν dxμdxν = − 2 ℓ 2 ds 2 AdS + 2 ds 2 S 3 , R (6) = 6 m 1/2 − supergravity fields, it is straightforward to derive the non-linear Kaluza-Klein reduction Ansätze for the various 6D fields. In the truncation to the common N = (1, 0) sector, the formulas consistently reduce to the reduction formulas from [12,15]. The results nicely illustrate the power of the ExFT framework as a tool in the study of consistent truncations. The three-dimensional scalar potentials allow for a number of stationary points, most of which, however, turn out to be unstable by the existence of scalar directions with negative mass squares below the Breitenlohner-Freedman bound. Interestingly, they admit a one-parameter family of non-supersymmetric but stable AdS 3 solutions. We have given the explicit uplift of this family to six dimensions. Further direct applications of our uplift formulas may include three-dimensional solutions with non-constant scalars such as holographic RG flows in the scalar potentials. On a more general note, the proof of the consistent truncation to particular three-dimensional gauged supergravities allows to consistently restrict holographic supergravity calculations such as [8][9][10][11] to a closed subsector of fields.
An immediate generalization of the results reported here is their extension to six-dimensional supergravities with additional tensor multiplet couplings which generically arise from reductions from ten dimensions. In the ExFT context this corresponds to an embedding SO(8, 4) ֒→ SO(8, 4 + n) of the exceptional field theories and the associated twist matrices. Upon working out the extended dictionary between ExFT and supergravity fields, the corresponding uplift formulas can be extracted in analogy to the results of this paper.
It would also be highly interesting to examine if similar techniques could be employed to construct consistent truncations involving higher massive Kaluza-Klein multiplets and leading to three-dimensional theories of the type constructed in [31]. This might require an extension of the present framework to more general embeddings in the spirit of [19,20].
Finally, it would be interesting to explore to which extent similar structures can be unveiled in the context of AdS 3 × S 2 truncations of the five-dimensional supergravities obtained from compactification of M-theory on Calabi-Yau three-manifolds.
The isometries of S 3 can be described in terms of the SO(4) Killing vectors Then the metric of the round S 3 can be written in the SO(4)-covariant form as Using these and the inverse metricg ij of the round S 3 , we find that which has proven to be of great value in the simplification of the uplift formulas throughout.
The following was also of use for the derivation of (5.10)