De Sitter–Schwarzschild metric

In general relativity, the de Sitter–Schwarzschild solution describes a black hole in a causal patch of de Sitter space. Unlike a flat-space black hole, there is a largest possible de Sitter black hole, which is the Nariai spacetime. The Nariai limit has no singularities, the cosmological and black hole horizons have the same area, and they can be mapped to each other by a discrete reflection symmetry in any causal patch.^[1][2][3]

Introduction

In general relativity, space-times can have black hole event horizons and also cosmological horizons. The de Sitter–Schwarzschild solution is the simplest solution which has both.

Metric

The metric of any spherically symmetric solution in Schwarzschild form is:

${\displaystyle ds^{2}=-f(r)dt^{2}+{dr^{2} \over f(r)}+r^{2}(d\theta ^{2}+\sin ^{2}\theta \,d\phi ^{2})\,}$ 

The vacuum Einstein equations give a linear equation for ƒ(r), which has as solutions:

${\displaystyle f(r)=1-2a/r\,}$ 

${\displaystyle f(r)=1-br^{2}\,}$ 

The first is a zero stress energy solution describing a black hole in empty space time, the second (with b positive) describes de Sitter space with a stress-energy of a positive cosmological constant of magnitude 3b. Superposing the two solutions gives the de Sitter–Schwarzschild solution:

${\displaystyle f(r)=1-{\frac {2a}{r}}-br^{2}\,}$ 

The two parameters a and b give the black hole mass and the cosmological constant respectively. In d + 1 dimensions, the inverse power law falloff in the black hole part is d − 2. In 2 + 1 dimensions, where the exponent is zero, the analogous solution starts with 2 + 1 de Sitter space, cuts out a wedge, and pastes the two sides of the wedge together to make a conical space.

The geodesic equation

${\displaystyle g_{aj}{\ddot {x}}^{j}+\left(\partial _{i}g_{aj}-{\frac {1}{2}}\partial _{a}g_{ij}\right){\dot {x}}^{j}{\dot {x}}^{i}=0\,}$ 

gives

${\displaystyle {\ddot {r}}+{\frac {1}{2}}{\frac {-f'(r)}{f(r)}}{\dot {r}}^{2}+{\frac {1}{2}}f(r)f'(r){\dot {t}}^{2}-rf(r){\dot {\theta }}-rf(r){\text{sin}}^{2}\theta {\dot {\phi }}^{2}=0}$ 

for the radial, and

${\displaystyle {\ddot {t}}+{\frac {1}{f(r)}}f'(r){\dot {t}}{\dot {r}}=0}$ 

for the time component.

Horizon properties

The de Sitter space is the simplest solution of Einstein's equation with a positive cosmological constant. It is spherically symmetric and it has a cosmological horizon surrounding any observer, and describes an inflating universe. The Schwarzschild solution is the simplest spherically symmetric solution of the Einstein equations with zero cosmological constant, and it describes a black hole event horizon in otherwise empty space. The de Sitter–Schwarzschild space-time is a combination of the two, and describes a black hole horizon spherically centered in an otherwise de Sitter universe. An observer which hasn't fallen into the black hole, and which can still see the black hole despite the inflation, is sandwiched between the two horizons.

In a semi-classical treatment, the de Sitter cosmological horizon can be thought of as absorbing or emitting depending on the point of view. Similarly, for a black hole that has been around for a long time, the horizon can be thought of as emitting or absorbing depending on whether you take the point of view of infalling matter or outgoing Hawking radiation. Hawking argued based on thermodynamics that the past horizon of a white hole is in fact physically the same as the future horizon of a black hole, so that past and future horizons are physically identical. This was elaborated by Susskind into black hole complementarity, which states that any interior parts of a black hole solution, in either the past and future horizon interpretation, can be holographically related by a unitary change of basis to the quantum mechanical description of the horizon itself.

The Nariai solution is the limit of the largest black hole in a space which is de Sitter at large distances, it has two horizons, the cosmological de Sitter horizon and a Schwarzschild black hole horizon. For small mass black holes, the two are very different--- there is a singularity at the center of the black hole, and there is no singularity past the cosmological horizon. But the Nariai limit considers making the black hole bigger and bigger, until its event horizon has the same area as the cosmological de Sitter horizon. At this point, the space-time becomes regular, the black hole singularity runs off to infinity, and the two horizons are related by a space-time symmetry.

In the Nariai limit, the black hole and de Sitter horizon can be interchanged just by changing the sign of the coordinate z. When there is additional matter density, the solution can be thought of as an Einstein spherical universe with two antipodal black holes. Whichever black hole becomes larger becomes the cosmological horizon.

Nariai solution

Starting with de Sitter–Schwarzschild:

${\displaystyle ds^{2}=-f(r)\,dt^{2}+{dr^{2} \over f(r)}+r^{2}(d\theta ^{2}+\sin ^{2}\theta \,d\phi ^{2})\,}$ 

with

${\displaystyle f(r)=1-{2a \over r}-br^{2}\,}$ 

The two parameters a and b give the black hole mass and the cosmological constant respectively. In higher dimensions, the power law for the black hole part is faster.

When a is small, ƒ(r) has two zeros at positive values of r, which are the location of the black hole and cosmological horizon respectively. As the parameter a increases, keeping the cosmological constant fixed, the two positive zeros come closer. At some value of a, they collide.

Approaching this value of a, the black hole and cosmological horizons are at nearly the same value of r. But the distance between them doesn't go to zero, because ƒ(r) is very small between the two zeros, and the square root of its reciprocal integrates to a finite value. If the two zeros of ƒ are at R + ε and R − ε taking the small ε limit while rescaling r to remove the ε dependence gives the Nariai solution.

The form of ƒ near the almost-double-zero in terms of the new coordinate u given by r = R + u is:

${\displaystyle f(r)={u^{2}-\epsilon ^{2} \over R^{2}}\,}$ 

The metric on the causal patch between the two horizons reduces to

${\displaystyle ds^{2}=-(R^{2}-z^{2})\,dt^{2}+{dz^{2} \over (R^{2}-z^{2})}+R^{2}\,d\Omega ^{2}\,}$ 

which is the metric of ${\displaystyle dS_{2}\times S_{2}}$ . This form is local for an observer sandwiched between the black hole and the cosmological horizon, which reveal their presence as the two horizons at z = −R and z = R respectively.

The coordinate z can be replaced by a global coordinate for the 1 + 1-dimensional de Sitter space part, and then the metric can be written as:

${\displaystyle dS^{2}=-dt^{2}+\cosh ^{2}t\,dx^{2}+R^{2}\,d\Omega ^{2}\,}$ 

In these global coordinates, the isotropy of de Sitter space makes shifts of the coordinate x isometries, so that it is possible to identify x with x + A, and make the space dimension into a circle. The constant-time radius of the circle expands exponentially into the future and the past, and this is Nariai's original form.

Rotating one of the horizons in Nariai space makes the other horizon rotate in the opposite sense. This is a manifestation of Mach's principle in self-contained causal patches, if the cosmological horizon is included as "matter", like its symmetric counterpart, the black hole.

Hawking temperature

The temperature of the small and large horizon in the de Sitter–Schwarzschild can be calculated as the period in imaginary time of the solution, or equivalently as the surface gravity near the horizon. The temperature of the smaller black hole is relatively larger, so there is heat flow from the smaller to the larger horizon. The quantity which is the temperature of the black hole is hard to define, because there is no asymptotically flat space to measure it relative to.

Curvature

The non-zero components of the Ricci curvature tensor for the de Sitter–Schwarzschild metric are

${\displaystyle R_{tt}={\frac {1}{2}}f(r)\left(2{\frac {f'(r)}{r}}+f''(r)\right)\,}$ 

${\displaystyle R_{rr}=-{\frac {2f'(r)+rf''(r)}{2rf(r)}}\,}$ 

${\displaystyle R_{\theta \theta }=1-f(r)-rf'(r)\,}$ 

${\displaystyle R_{\phi \phi }=-\sin ^{2}(\theta )\left(-1+f(r)+rf'(r)\right)\,}$ 

and the Ricci curvature scalar

${\displaystyle R={\frac {2-2f(r)-4rf'(r)-r^{2}f''(r)}{r^{2}}}\,}$ 

See also

• De Sitter space
• Anti-de Sitter space
• De Sitter universe
• Kerr–Newman–de–Sitter metric
• AdS/CFT correspondence

References

1. R. Bousso (2003). "Adventures in de Sitter space". In G. W. Gibbons; E. P. S. Shellard; S. J. Rankin (eds.). The future of theoretical physics and cosmology. Cambridge University Press. pp. 539–569. arXiv:hep-th/0205177. Bibcode:2003ftpc.book..539B. ISBN 978-0-521-86015-4.
2. H. Nariai (1950). "On some static solutions of Einstein's gravitational field equations in a spherically symmetric case". Sci. Rep. Tohoku Univ. 34: 160.
3. H. Nariai (1951). "On a new cosmological solution of Einstein's field equations of gravitation". Sci. Rep. Tohoku Univ. 35: 62.