AdS2 × S7 solutions from D0-F1-D8 intersections

We study an exhaustive analytic class of massive type IIA backgrounds pre-serving sixteen real supercharges and enjoying SL(2, ℝ) × SO(8) bosonic symmetry. The corresponding geometry is described by AdS2 × S7 warped over a line, which turns out to emerge from taking the near-horizon limit of D0-F1-D8 intersections. By studying the singularity structure of these solutions we find the possible presence of localized O8/D8 sources, as well as of fundamental strings smeared over the S7. Finally we discuss the relation between the aforementioned solutions and the known AdS7 × S2 class through double analytic continuation.

The paper is organized as follows. We start out by reviewing some facts concerning D0-F1-D8 intersections in massive type IIA string theory and relate them to 1 4 -BPS supergravity solutions discussed in [10]. Subsequently, we show how to make an educated guess in the general Ansatz which directly produces solutions with enhanced supersymmetry thus realizing AdS 2 geometry. After integrating the obtained differential equations, we discuss the relation of the obtained solutions to the aforementioned AdS 7 counterparts through double analytic continuation. Then, we discuss the possible singularity structures as well as the range of the warp coordinate. We conclude with some further speculations concerning the possible holographic interpretation of our work.
2 AdS 2 solutions from D0-F1-D8 intersections D0-D8 bound states were considered in [11][12][13][14] as UV descriptions of N = (8, 0) superconformal quantum mechanics. Such bound states require a non-trivial B-field sourced by a fundamental string. Note that, contrary to all other D-branes, strings cannot end on a D-particle due to charge conservation issues [15,16]. However the situation changes in presence of D8-branes in the background, where in fact an F1 stretched between a D0 and the D8 has to be formed whenever the D0 crosses a D8 [17]. This physical process can be understood as a dual version of the Hanany-Witten (HW) effect [18].
D0-F1-D8 brane systems were exhaustively studied in [10,19] as a class of 1 4 -BPS solutions in massive type IIA supergravity. The explicit set-up is summarized in table 1.
The complete Ansatz for the 10D fields of massive type IIA supergravity can be completely specified in terms of two arbitrary functions of the (y, r) coordinates, denoted by S & K. This reads where g s > 0 is the string coupling and dΩ 2 (7) denotes the metric of a unit-radius sevensphere.

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For non-zero Romans' mass m the full set of 10D equations of motion and Bianchi identities is implied by the following non-linear PDE's where ∆ (8) is the Laplace operator on R 8 , i.e. the common transeverse space to the Dparticle and the string. Its rotationally invariant form expressed in polar coordinates reads Note that in the massless limit K is no longer determined by the equation (2.2a), but it must instead satisfy the following PDE A particular solution to (2.2b) & (2.4) is given by the semilocalized D0-F1 intersection constructed by following the prescription in [20], this procedure yielding In the remaining part of this section we will show how to extract massive AdS 2 solutions from the PDE's (2.2a) & (2.2a). We will follow the same procedure illustrated in [21], where the AdS 7 solutions of [7] are seen as emerging from NS5-D6-D8 systems of the Hanany-Zaffaroni type [22]. The key will be understanding which combination of the (y, r) coordinates plays the role of the radial coordinate of AdS 2 , thus transforming the original system of PDE's determining 1 4 -BPS flows into a single ODE yielding warped AdS geometries with enhanced supersymmetry as solutions. Analog to the case studied in [21], we will be able to exploit the insight coming from the massless case also when the Romans' mass is turned on. This will result in an exhaustive classification of all AdS 2 of this type in massive type IIA string theory.
The near-horizon limit of the D0-F1 system. Let us first start from the massless solution in (2.5) describing the semilocalized intersection between a D-particle and a fundamental string. By performing the following coordinate change [23]

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we find that the metric, in the ρ → 0 limit, takes the form , which is the warped product of AdS 2 and an 8-manifold obtained as a fibration of S 7 over a line. The insight that we can borrow from the massless situation described above is that taking the near-horizon limit where AdS emerges, involves the following two conditions In the following part of this section we will make use of the above conditions in order to guess the change of variables that translates the PDE's in (2.2a) & (2.2b) into a single ODE to be solved for AdS solutions.
AdS 2 × S 7 solutions in massive type IIA supergravity. Inspired by (2.9), we proceed by making the following Ansatz for the S and K functions where G is an arbitrary function of the combination y 2 r 4 ≡ ζ, and κ is a constant yet to be determined. For the above choice of S & K the dilaton reads which stays finite in the limit (2.9) only when κ = −6. With this choice for κ, the 10D metric turns out to be given by AdS 2 × S 7 warped over the ζ coordinate, the warping being specified by the function G(ζ). Upon introducing new coordinates defined by one can furthermore check that the full set of equations of motion and Bianchi identities are implied whenever G satisfies the following ODE where a prime denotes differentiation with respect to ζ. This is solved by where γ 1 & γ 2 are integration constants. The metric now becomes where we recognize ds 2 2 as the line element of AdS 2 of radius 1/4. Note that the above solution may be trusted as a good supergravity solution since it admits the g s ≪ 1 limit, in which the string dilaton becomes small while the overall warp factor grows large in string units.
Relation to AdS 7 × S 2 through double analytic continuation. From the previous analysis it appears evident that our class of AdS 2 solutions realizes the superalgebra osp(8|2) as an isometry algebra, just like the AdS 7 ones in [7,8]. The only difference between the two realizations being the different choice of real form, i.e. so(2, 1) ⊕ so (8) for AdS 2 vs. so(2, 6) ⊕ so(3) for AdS 7 . A similar phenomenon has been recently discussed in [9] for AdS 6 × S 2 vs. AdS 2 × S 6 solutions of type IIB supergravity, where in both cases the aforementioned 8-dimensional geometry is warped over a Riemann surface Σ. There it was argued that the two geometries are related by a so-called double analytic continuation involving an interchange of AdS and sphere factors, while at the same time performing a Wick rotation of the coordinate parametrizing the warping.
In order to make a similar relation manifest for our case, we introduce a new coordinate z and a suitable function α(z) such that where a dot denotes differentiation with respect to z. The ODE (2.14) for G then becomes the following one for α ....
which is solved cubic polynomials in z of the form The metric now becomes , (2.20) where ds 2 AdS 2 is the line element of AdS 2 of unit radius and The dilaton reads e Φ = g s ℓ 3 α α We recognize the above metric as the double analytic continuation of the AdS 7 solution of [7,8]  Let us note that although the above solution is obtained in massive type IIA supergravity, we can get the massless limit by taking m → 0 and c 3 → 0 at the same time. Hence we will discuss the massless solution separately.

JHEP10(2018)190 3 Analysis of the solutions
In this section we analyze the geometry and the dilaton of the solution. To this end, it turns out to be very convenient to use the z coordinate that directly relates our solutions to the AdS 7 ones in [24]. We keep c 3 = 0 as in the opposite case we would obtain a massless solution, as mentioned in the end of the previous section.
Positivity of the metric (2.20) metric requires The special loci of the geometry, where the warp factor vanishes or tends to infinity are (i) α = 0, or (ii)α = 0, or (iii)α 2 − 2αα = 0. Note that, in particular, positivity of the metric requiresα going to zero, whenever either α orα go to zero. Hence we have the following special loci: • a double root of α • a triple root of α • a root ofα andα (stationary point of inflection of α) • a root ofα 2 − 2αα, while keepingα = 0 &α = 0 The discriminant ofα 2 − 2αα is ∆(α 2 − 2αα) = −2 8 3 3 c 2 3 ∆(α) 2 , hence we only need to consider a simple root ofα 2 −2αα as a multiple root is also a multiple root of α and this is covered by the first two cases. In particularα 2 − 2αα can have simple roots, a triple root wich corresponds to a double root of α, or a quadruple root which corresponds to triple root of α.
Let us now analyze the geometry and the dilaton near the aforementioned loci.
• Near a double root z 0 of α the metric reads where ̺ 2 ≡ z − z 0 , and the dilaton stays finite. Hence the internal space becomes R 8 and the geometry is regular.
• Near a triple zero the metric becomes .

(3.3)
Then we recognize this as a conical singularity. Its physical interpretation as arising from an orbifold is not clear and hence we will dismiss this case.
• Near a stationary point of inflection of α the metric reads The dilaton becomes This singularity we recognize as an O8/D8-brane singularity.
We now look at the range of z. An analysis of the roots of the quartic polymialα 2 −2αα shows that it always has two real roots (simple or multiple). Since the coefficient of the z 4 term ofα 2 − 2αα is −3c 2 3 , we conclude that it stays negative for z ∈ [z 0 , ∞] where z 0 is a root. The behavior of the solution at infinity is , and for the dilaton ℓ −3 e Φ ∼ β 4 z −1/2 , with β 4 a constant.
It is worth mentioning that such a behavior at infinity can be understood as that of a curved D8-domain wall carrying D0-brane charge. This type of BI-on solutions was also investigated in [10]. To make our claim manifest, we describe our asymptotic solution at ∞ as which corresponds to picking G ∞ = 4 3 ζ, and interpret it as a curved domain wall solution whose profile is described by which for S = S ∞ integrates to y = c r 2/3 . One can then check that the metric (3.7) is reproduced by the following change of coordinates where R is to be identified with the AdS 2 radial coordinate.
Compactifying the range of the warp coordinate. Although z is defined on a halfline we can compactify it by making a coordinate tranformation to a trigonometric function. Let us look at the case where α has a double root, in the neighborhood of which the internal space is regular. We thus take and perform the following coordinate transformation (3.11) The metric then becomes ℓ −2 ds 2 10 = |z 0 − z 1 | √ 2 sec 2 θ 1 + 2 sin 2 θ 1 4 1 + 2 sin 2 θ 4 − sin 2 θ ds 2 AdS 2 + 1 + 2 sin 2 θ cos 2 θ dθ 2 + sin 2 θdΩ 2 (7) .

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The massless solution. In the massless limit we need to take c 3 = 0 and so α becomes a quadratic polynomial.α 2 − 2αα evaluates to c 2 1 − 4c 0 c 2 which is also the discriminant of ∆(α) of α. Sinceα 2 − 2αα has to be negative we conclude that α has complex roots and is always different from zero. The metric now reads . (3.13) Upon making the following coordinate transformation 14) The metric takes exactly the form in (2.8) obtained as the near-horizon geometry of the massless D0-F1 semilocalized intersection in [23, section 4.5], provided that Q D0 ≡ 1

Conclusions
In this paper we have studied a class of warped supersymmetric AdS 2 solutions in massive type IIA emerging from D0-F1-D8 systems as their near-horizon geometries. All solutions in this class turn out to preserve sixteen real supercharges and the corresponding internal geometry is given by a fibration of a (round) seven-sphere over a line.
The solutions can be on the one hand obtained as special cases of the 1 4 -BPS family of backgrounds studied in [10], and on the other hand reinterpreted as the double-analytically continued version of the AdS 7 solutions of [7,8]. This latter relation is further corroborated by the fact that both families offer explicit realizations of the osp(8|2) superalgebra within massive type IIA supergravity, their distinction just corresponding to different choices of real form.
Due to the corresponding brane picture of the vacua discussed here, we expect them to be dual to some N = (8, 0) superconformal quantum mechanics. The first interesting check for a possible AdS 2 /CFT 1 correspondence in this context would be to be able to compute the holographic central charge by following the prescription where both the effective AdS radius L AdS and the Newton constant G (d+1) N are averaged over the warping, and make sense of the answer from a field theory viewpoint.
However, it may be worth mentioning that the above prescription for computing c hol would yield an infinite result in our case. This is mainly due to the range of the z warp coordinate being non-compact. Similar pathologies where also encountered in [25,26] in the context of AdS 5 solutions in type IIA obtained by taking a non-Abelian T-duality (NATD) on the type IIB Klebanov-Witten AdS 5 × T 1,1 background [27]. There this issue was resolved on the gravity side by introducing a hard cut-off which should be interpreted JHEP10(2018)190 from a physical perspective as inserting the suitable branes which interrupt the dual quiver which would otherwise be infinitely long.
It would be interesting to investigate whether this feature that our solutions have, can be resolved in a way similar to the NATD solutions. This could possibly shed a light on their holographic dual superconformal quantum mechanical models and the possible emergence of deconstructed extra dimensions underlying this structure. We hope to come back to these issues in the future.