Abstract
The inverse scattering method of Belinsky and Zakharov is a powerful method to construct solutions of vacuum Einstein equations. In particular, in five dimensions this method has been successfully applied to construct a large variety of black hole solutions. Recent applications of this method to Einstein–Maxwell-dilaton (EMd) theory, for the special case of Kaluza–Klein dilaton coupling, has led to the construction of the most general black ring in this theory. In this contribution, we review the inverse scattering method and its application to the EMd theory. We illustrate the efficiency of these methods with a detailed construction of an electrically charged black ring.





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In Ref. [30] a further reduction to 2D was considered, and the fruitful intertwining of this solution-generating technique with the ISM was studied. The ISM from the point of view of two dimensional symmetries has also been recently investigated in [33]. Hidden symmetries have also been employed in [34, 35] to obtain charged black rings in other theories, following the pioneering work [36].
As we explain in Sect. 3 the conformal factor is completely specified by the Killing metric. Hence the information contained in the rod structure is enough to fully reconstruct the line element.
The operation of removing a (anti-)soliton is the inverse of adding a (anti-)soliton. For a diagonal seed it is easy to show that removing a (anti-)soliton \(\widetilde{\mu }_i\) with a trivial BZ vector of the form \((m_0)_a=\delta _{ab}\) simply results in multiplying \((G_0)_{bb}\) by \(-\widetilde{\mu }_i^2/\rho ^2\), leaving the remaining components invariant.
However, note that to correctly generate the dipole ring from the seed of Fig. 3 one must remove and add anti-solitons at \(z=a_0\) and \(z=a_2\), whereas for the construction we present here we will apply a solitonic transformation at \(z=a_0\) and \(z=a_4\).
Generically, after such solitonic transformations one is not guaranteed to obtain a final metric with standard orientation, i.e., with the semi-infinite rods coinciding with the \(\phi \) and \(\psi \) directions. This can be remedied by making a coordinate transformation, \(\mathbf G \rightarrow \tilde{\mathbf{G }}=\mathbf S ^T \mathbf G \, \mathbf S \) with \(\mathbf S \in SL(4,\mathbb R )\). However, the construction discussed in this paper requires no coordinate mixing and so the matrix \(\mathbf S \) is trivial.
The solution is invariant under an overall shift in \(z\) so we subtract 1 from the total number of \(a_i\)’s.
We adopt the standard definition for an electric charge in \(D\) dimensions, normalizing by the area of the unit \((D-2)\)-sphere. For \(D=5\) we get \(Q_e=\frac{1}{2\pi ^2}\int _{S_\infty ^3}*F\).
The explicit transformation of the coordinates and parameters that takes our solution (54–56) to the Kunduri-Lucietti charged ring is given by
$$\begin{aligned} t&= \hat{t}\,, \quad (\psi ,\phi )=\frac{1+\hat{\nu }(1-k^2)}{\sqrt{1+\hat{\lambda }}}(\hat{\psi },\hat{\phi })\,, \quad x=\frac{\hat{x}-\hat{\lambda }}{1-\hat{\lambda }\hat{x}}\,, \quad y=\frac{\hat{y}-\hat{\lambda }}{1-\hat{\lambda }\hat{y}}\,,\end{aligned}$$(57)$$\begin{aligned} \lambda&= \hat{\lambda }\,, \quad \nu =\frac{\hat{\lambda }-\hat{\nu }(1-k^2)}{1-\hat{\lambda }\hat{\nu }(1-k^2)}\,, \quad \gamma =\frac{k^2 \hat{\lambda }}{1-k^2}\,, \quad R=\frac{\sqrt{(1+\hat{\lambda })\left( 1-\hat{\lambda }\hat{\nu } (1-k^2)\right) }}{1+\hat{\nu } (1-k^2)}\hat{R}\,, \end{aligned}$$(58)where hatted quantities correspond to coordinates and parameters employed in Ref. [41]. We note in passing that Eqs. (39) and (40) of Ref. [41] contain small typos.
The family of solutions obtained in Ref. [40] generically have non-vanishing \(S^2\) angular momentum and dipole charge. Setting these quantities to zero corresponds to taking the limit \(\mu \rightarrow 0\) while keeping \(a_1\) finite, in the notation of [40]. The resulting solution is parametrized by three numbers \((k, c, a_3)\) and the comparison with the explicit solution constructed in this paper may be done employing the following relations between parameters:
$$\begin{aligned} R^2 = \frac{2}{1+c^2}k^2\,, \qquad \gamma = \frac{8 a_3^2 c^3}{(1+c^2)[(1-c^2)^2-4 a_3^2 c^2]}\,, \qquad \nu = c\,. \end{aligned}$$(67)Special care must be taken when comparing the formulas for the electric charge and potential: the normalization adopted in [40] differs from ours by a multiplicative factor of \(\pi /16\).
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Acknowledgments
We thank James Lucietti for bringing Ref. [41] to our attention, and Axel Kleinschmidt for a comment on the draft. J.V.R. is supported by Fundação para a Ciência e Tecnologia (FCT)—Portugal through contract no. SFRH/BPD/47332/2008. M.J.R. is supported by the European Commission—Marie Curie grant PIOF-GA 2010-275082. O.V. is supported in part by the Netherlands Organisation for Scientific Research (NWO) under the VICI grant 680-47-603. A.V. thanks IUCAA Pune for hospitality where part of this work was done.
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This article belongs to the Topical Collection: Progress in Mathematical Relativity with Applications to Astrophysics and Cosmology.
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Rocha, J.V., Rodriguez, M.J., Varela, O. et al. Charged black rings from inverse scattering. Gen Relativ Gravit 45, 2099–2121 (2013). https://doi.org/10.1007/s10714-013-1586-x
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DOI: https://doi.org/10.1007/s10714-013-1586-x