The coset structure of the stationary field equations is shared by various self-gravitating matter models with massless scalars (moduli) and Abelian vector fields. For scalar mappings into a symmetric target space , say, Breitenlohner et al.  have classified the models admitting a symmetry group which is sufficiently large to comprise all scalar fields arising on the effective level48 within one coset space, . A prominent example of this kind is the EM-dilaton-axion system, which is relevant to supergravity and to the bosonic sector of four-dimensional heterotic string theory: The pure dilaton-axion system has an symmetry which persists in dilaton-axion gravity with an Abelian gauge field . Like the EM system, the model also possesses an symmetry, arising from the dimensional reduction with respect to the Abelian isometry group generated by the Killing field. Gal’tsov and Kechkin [63, 64] have shown that the full symmetry group is, however, larger than : The target space for dilaton-axion gravity with an vector field is the coset . Using the fact that is isomorphic to , Gal’tsov and Kechkin  were also able to give a parametrization of the target space in terms of (rather than ) matrices. The relevant coset was shown to be .49
Common to the black hole solutions of the above models is the fact that their Komar mass can be expressed in terms of the total charges and the area and surface gravity of the horizon . The reason for this is the following: Like the EM equations (32), the stationary field equations consist of the three-dimensional Einstein equations and the -model equations,50 The crucial observation is that Stokes’ theorem provides independent Smarr relations, rather than only ones. (This is due to the fact that all -model currents are algebraically independent, although there are differential identities which can be derived from the field equations.)
The complete set of Smarr type formulas can be used to get rid of the horizon-values of the scalar potentials. In this way one obtains a relation which involves only the Komar mass, the charges and the horizon quantities. For the EM-dilaton-axion system one finds, for instance ,51
A very simple illustration of the idea outlined above is the static, purely electric EM system. In this case, the electrovac coset reduces to . The matrix is parametrized in terms of the electric potential and the gravitational potential . The -model equations comprise differential conservation laws, of which is redundant:52 additional relation of the Smarr type,
In the “extreme” case, the BPS bound  for the static EM-dilaton-axion system, , was previously obtained by constructing the null geodesics of the target space . For spherically symmetric configurations with non-degenerate horizons (), Eq. (37) was derived by Breitenlohner et al. . In fact, many of the spherically symmetric black hole solutions with scalar and vector fields [72, 76, 69] are known to fulfill Eq. (37), where the LHS is expressed in terms of the horizon radius (see  and references therein). Using the generalized first law of black hole thermodynamics, Gibbons et al.  recently obtained Eq. (37) for spherically symmetric solutions with an arbitrary number of vector and moduli fields.
The above derivation of the mass formula (37) is neither restricted to spherically symmetric configurations, nor are the solutions required to be static. The crucial observation is that the coset structure gives rise to a set of Smarr formulas which is sufficiently large to derive the desired relation. Although the result (37) was established by using the explicit representations of the EM and EM-dilaton-axion coset spaces , similar relations are expected to exist in the general case. More precisely, it should be possible to show that the Hawking temperature of all asymptotically flat (or asymptotically NUT) non-rotating black holes with massless scalars and Abelian vector fields is given bysymmetric space, . Here and denote the charges of the scalars (including the gravitational ones) and the vector fields, respectively.
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