Upper bound on the radii of black-hole photonspheres

TL;DR

This paper establishes an upper limit on the radius of photonspheres in spherically symmetric black-hole spacetimes, showing that it cannot exceed three times the black hole's mass, with implications for hairy black holes.

Contribution

It proves a universal upper bound on photonsphere radii in spherically symmetric asymptotically flat black holes, including hairy black holes, extending previous results.

Findings

Photonsphere radius is bounded by 3 times the black hole mass.

The Schwarzschild black hole saturates this bound.

Hairy black holes also conform to this upper limit.

Abstract

One of the most remarkable predictions of the general theory of relativity is the existence of black-hole "photonspheres", compact null hypersurfaces on which massless particles can orbit the central black hole. We prove that every spherically-symmetric asymptotically flat black-hole spacetime is characterized by a photonsphere whose radius is bounded from above by $r_{\gamma} \leq 3M$, where $M$ is the total ADM mass of the black-hole spacetime. It is shown that hairy black-hole configurations conform to this upper bound. In particular, the null circular geodesic of the (bald) Schwarzschild black-hole spacetime saturates the bound.

Equations

$$d{s}^2=-e^{-2\delta }\mu d{t}^2+{\mu }^{-1}d{r}^2+r^2(d{\theta }^2+{\sin }^2\theta d{\varphi }^2),$$

$$\mu (r\to \infty )\to 1\text{and}\delta (r\to \infty )\to 0.$$

$${\mu }^{\prime }=-8\pi r\rho +(1-\mu )/r,$$

$${\delta }^{\prime }=-4\pi r(\rho +p)/\mu ,$$

$$\mu (r_{\text{H}})=0\text{with}{\mu }^{\prime }(r_{\text{H}})\ge 0,$$

$$\delta (r_{\text{H}})<\infty ;{\delta }^{\prime }(r_{\text{H}})<\infty .$$

$$8\pi r_{\text{H}}^2\rho (r_{\text{H}})\le 1.$$

$$-p(r_{\text{H}})=\rho (r_{\text{H}}).$$

$$m(r)=\frac{1}{2}{r}_{\text{H}}+{\int }_{r_{\text{H}}}^{r}4\pi r^{\prime 2}\rho (r^{\prime })d{r}^{\prime },$$

$$\mu (r)\equiv 1-2m(r)/r.$$

$$r^3\rho (r)\to 0\text{as}r\to \infty .$$

$$2\mathcal{L}=-e^{-2\delta }\mu {\dot{t}}^2+{\mu }^{-1}{\dot{r}}^2+r^2{\dot{\varphi }}^2,$$

$$p_t=-e^{-2\delta }\mu \dot{t}\equiv -E=\text{const},$$

$$p_{\varphi }=r^2\dot{\varphi }\equiv L=\text{const},$$

$$p_r={\mu }^{-1}\dot{r}.$$

$$2\mathcal{H}=-E\dot{t}+L\dot{\varphi }+{\mu }^{-1}{\dot{r}}^2=ϵ=\text{const},$$

$$\dot{r}^{2}=\mu\Big{(}{{E^{2}}\over{e^{-2\delta}\mu}}-{{L^{2}}\over{r^{2}}}\Big{)}\$$

$$2e^{-2\delta}\mu-r(e^{-2\delta}\mu)^{{}^{\prime}}=0\$$

$${\cal N}(r=r_{\gamma})=0\$$

$$\mathcal{N}(r)\equiv 3\mu -1-8\pi r^{2}p.$$

$${\cal N}(r_{\text{H}})\leq 0\$$

$$\mathcal{N}(r\to \infty )\to 2.$$

$$\mathcal{N}(r_{\text{H}}\le r<r_{\gamma })<0.$$

$$T_{r;\mu }^{\mu }=0.$$

$$\displaystyle p^{\prime}(r)={{1}\over{2\mu r}}\big{[}(3\mu-1-8\pi r^{2}p)(\rho+p)+2\mu T-8\mu p\big{]}\ ,$$

$$P^{\prime }(r)$$

$$\rho \ge 0,$$

$$\rho +p\ge 0.$$

$$T\le 0.$$

$$P(r_{\text{H}})\le 0.$$

Full text

I Introduction

The geodesic motions of test particles around central compact objects (e.g. black holes, neutron stars) provide valuable information about the structure and geometry of the corresponding curved spacetime Bar ; Chan ; Shap ; CarC . Of particular importance are circular null geodesics – orbits with constant coordinate radii on which massless particles can orbit the central compact object Notebn . Circular null orbits (also known as “photon orbits” or “photonspheres”) are interesting from both an astrophysical and theoretical points of view Bar ; Chan ; Shap ; CarC ; Hodns . For example, the optical appearance to external observers of a compact star undergoing gravitational collapse is closely related to the physical properties of the photonsphere CarC ; Pod ; Ame .

Unstable circular null geodesics are also related to the characteristic (quasinormal) resonances of black-hole spacetimes CarC ; Mash ; Goeb ; Hod1 ; Dolan ; Dec ; Yang . In particular, in the framework of the geometric-optics (eikonal) approximation, these characteristic resonances can be interpreted in terms of massless particles temporarily trapped at the unstable null orbit of the black-hole spacetime CarC ; Mash ; Goeb ; Hod1 ; Dolan ; Dec ; Yang . In addition, it was shown Ste that the remarkable phenomenon of strong gravitational lensing by black holes is closely related to the presence of null circular geodesics in the corresponding black-hole spacetimes.

Furthermore, for hairy black-hole spacetimes a theorem was recently proved Hodhair ; Nun that reveals the central role played by the black-hole photonsphere in determining the effective length of the hair outside the black-hole horizon. According to this theorem, the non-trivial (non-asymptotic) behavior of the hair must extend above the black-hole photonsphere. In this respect, the black-hole photonsphere provides a generic lower bound on the effective length of the black-hole hair Hodhair ; Nun . In addition, it was recently proved Hodfast that the innermost null circular geodesic of a black-hole spacetime provides the fastest way (as measured by asymptotic observers) to circle the central black hole.

The central role played by photonspheres in both astrophysical CarC ; Pod ; Ame and cosmological Ste scenarios involving black holes, as well as in purely theoretical studies of black-hole spacetimes CarC ; Mash ; Goeb ; Hod1 ; Dolan ; Dec ; Yang ; Hodhair ; Hodfast , makes it highly important to explore the physical properties of these unique null orbits. The main goal of the present study is to extend our knowledge about the physical properties of these fascinating geodesics. In particular, in the present paper we shall address the following question: In a generic black-hole spacetime, how close is the photonsphere to the black-hole horizon? As we shall show below, one can derive a generic upper bound on the radii of black-hole photonspheres. This bound is expressed in terms of the total (ADM) mass of the black-hole spacetime.

II Description of the system

We consider static, spherically symmetric, asymptotically flat black-hole spacetimes. The line element may take the following form in Schwarzschild coordinates Nun ; Hodfast ; Hodm

[TABLE]

where the metric functions $\delta(r)$ and $\mu(r)$ depend only on the Schwarzschild areal coordinate $r$. Asymptotic flatness requires

[TABLE]

It is worth emphasizing that our results would be valid for all spherically symmetric asymptotically flat black-hole spacetimes. We note, in particular, that we do not assume $\delta(r)=0$ (a property which characterizes the familiar Schwarzschild and Reissner-Nordström black-hole spacetimes) and thus our results would be applicable to hairy black-hole configurations as well [in these spacetimes $\delta(r)\neq 0$, see BizCol ; Lavr ; Green ; Stra ; Volkov and references therein].

Taking $T^{t}_{t}=-\rho$, $T^{r}_{r}=p$, and $T^{\theta}_{\theta}=T^{\phi}_{\phi}=p_{T}$, where $\rho$, $p$, and $p_{T}$ are identified as the energy density, radial pressure, and tangential pressure respectively Bond1 , the Einstein equations $G^{\mu}_{\nu}=8\pi T^{\mu}_{\nu}$ read

[TABLE]

and

[TABLE]

where the prime stands for differentiation with respect to $r$. (We use natural units in which $G=c=1$.)

Regularity of the event horizon at $r=r_{\text{H}}$ requires Nun

[TABLE]

and

[TABLE]

From Eqs. (3) and (5) one finds the boundary condition Bekreg ; Nun

[TABLE]

The equality sign corresponds to extremal black holes. From Eqs. (4)-(6) one finds the additional boundary condition

[TABLE]

The mass $m(r)$ contained within a sphere of radius $r$ is given by

[TABLE]

where $m(r_{\text{H}})=r_{\text{H}}/2$ is the horizon mass. From Eqs. (3) and (9) one finds the relation

[TABLE]

A finite mass configuration is characterized by a density profile $\rho(r)$ which approaches zero faster than $r^{-3}$,

[TABLE]

III Upper bound on the radii of black-hole photonspheres

We shall now consider the following question: In the generic spherically-symmetric black-hole spacetime (1), how close is the photonsphere to the black-hole horizon? To answer this question in the most general form, we shall now prove the existence of a generic upper bound on the radius of the innermost null circular geodesic.

We shall first follow the analysis of Chan ; CarC ; Hodhair ; Hodfast in order to calculate the location $r=r_{\gamma}$ of the null circular geodesic for a black-hole spacetime described by the line element (1). The Lagrangian describing the geodesics in the spacetime (1) is given by

[TABLE]

where a dot stands for differentiation with respect to proper time.

The generalized momenta derived from the Lagrangian (12) are given by Chan ; CarC

[TABLE]

[TABLE]

and

[TABLE]

The Lagrangian is independent of both $t$ and $\phi$. This implies that $E$ and $L$ are constants of the motion. The Hamiltonian of the system is given by Chan ; CarC ${\cal H}=p_{t}\dot{t}+p_{r}\dot{r}+p_{\phi}\dot{\phi}-{\cal L}$, which implies

[TABLE]

where $\epsilon=0$ for null geodesics and $\epsilon=1$ for timelike geodesics. Substituting Eqs. (13)-(14) into (16), one finds

[TABLE]

for null geodesics.

Circular geodesics are characterized by $\dot{r}^{2}=(\dot{r}^{2})^{{}^{\prime}}=0$ Chan ; CarC . This yields the relation

[TABLE]

for the null circular geodesic. Substituting the Einstein equations (3)-(4) into Eq. (18), one finds the characteristic relation

[TABLE]

for null circular orbits, where

[TABLE]

We shall henceforth consider the innermost circular null geodesic of the black-hole spacetime. Of course, this geodesic must satisfy the characteristic equation (19). We shall first prove that such circular null geodesic must exist in the black-hole spacetime: taking cognizance of Eqs. (5), (7), (8), and (20), one finds

[TABLE]

at the black-hole horizon Noteex . In addition, from Eqs. (2), (11), and (20) [see also Eq. (28) below] one finds the asymptotic behavior

[TABLE]

Inspection of Eqs. (21) and (22) reveals that there must be at least one intermediate radius $r_{\gamma}$ (located between the black-hole horizon and spatial infinity) for which ${\cal N}(r=r_{\gamma})=0$. This radius corresponds to the location of the null circular geodesic, see Eq. (19).

It is worth emphasizing that the null circular geodesic (19) is the limiting case of timelike circular geodesics. That is, the null circular geodesic is the innermost circular orbit in the black-hole spacetime Chan ; CarC . The spacetime region between the black-hole horizon and the photonsphere, $r_{\text{H}}\leq r<r_{\gamma}$, in which circular geodesics are excluded, is characterized by the inequality

[TABLE]

We shall now derive a generic upper bound on the radii of the innermost null circular geodesics. The conservation equation $T^{\mu}_{\nu;\mu}=0$ for the energy-momentum tensor has only one nontrivial component Nun

[TABLE]

Substituting Eqs. (3) and (4) into Eq. (24), one finds for the pressure gradient

[TABLE]

where $T=-\rho+p+2p_{T}$ is the trace of the energy momentum tensor. Below we shall analyze the behavior of the pressure function $P(r)\equiv r^{4}p(r)$, whose derivative is given by

[TABLE]

When analyzing the coupled Einstein-matter system, one usually imposes some energy conditions on the matter fields. We shall assume that the hair (the matter fields) outside the black-hole horizon satisfies the following conditions:

(1) The weak energy condition (WEC). This means that the energy density is positive semidefinite,

[TABLE]

and that it bounds the pressures. In particular, $|p|\leq\rho$. This implies the inequality

[TABLE]

(2) The trace of the energy-momentum tensor plays a central role in determining the spacetime geometry of compact objects Bond1 . It is usually assumed to satisfy the relation $p+2p_{T}\leq\rho$ (see Bond1 and references therein), which implies

[TABLE]

It is worth emphasizing that the two conditions (28) and (29) are indeed satisfied in all Einstein-matter models in which hairy black-hole configurations have been found (see Nun for details).

From Eqs. (8) and (27) one finds the boundary condition

[TABLE]

Furthermore, taking cognizance of the pressure gradient (26), together with the energy conditions (28) and (29), and the characteristic inequality (23), one finds

[TABLE]

below the photonsphere.

Combining the two inequalities (30) and (31), one concludes that $P(r)$ is a non-positive and decreasing function in the spacetime region below the photonsphere. In particular,

[TABLE]

at the null circular geodesic. Substituting (32) into the characteristic equations (19)-(20) for the null circular geodesic, one finds

[TABLE]

which implies [see Eq. (10)]

[TABLE]

Finally, from Eqs. (9), (27), and (34) one obtains the upper bound

[TABLE]

where $M\equiv m(r\to\infty)$ is the total (ADM) mass of the black-hole spacetime.

IV Summary and discussion

The characteristic photonspheres of spherically-symmetric black-hole spacetimes were studied analytically within the framework of the general theory of relativity. In particular, we have proved the existence of a generic upper bound on the radii of the innermost black-hole null circular geodesics [see Eq. (35)]. This bound is expressed in terms of the total ADM mass of the black-hole spacetime. It was shown that hairy black-hole configurations conform to this upper bound. Remarkably, the generic bound (35) is saturated by the null circular geodesic of the (bald) Schwarzschild black-hole spacetime.

Finally, it is worth mentioning that black-hole photonspheres are closely related to the characteristic quasinormal resonances of the corresponding black-hole spacetimes CarC ; Mash ; Goeb ; Hod1 ; Dolan ; Dec ; Yang . In particular, in the eikonal (geometric-optics) limit, the real parts of the resonances are given by the simple relation CarC

[TABLE]

Here $\Omega_{\infty}$ is the angular velocity (as measured by asymptotic observers) associated with the null circular geodesic of the black-hole spacetime, and $m\gg 1$ is the azimuthal quantum number of the perturbation mode. The angular velocity as measured by asymptotic observers, $\Omega_{\infty}$, is given by Hodfast

[TABLE]

The nominator of Eq. (37) represents the red-shift factor $g^{1/2}_{tt}$ due to the presence of the central black hole [see Eq. (1)]. Using the inequality $\mu(r_{\gamma})\leq{1/3}$ which characterizes the black-hole photonsphere [see Eq. (33)], together with the inequalities $\delta\geq 0$ Notedel and $r_{\gamma}\geq r_{\text{H}}$, one finds from (37) the upper bound

[TABLE]

on the dimensionless angular velocity associated with the null circular geodesic of the black-hole spacetime. This bound, together with the relation (36) between the real parts of the black-hole resonances and the angular velocity at the null circular geodesic, yield the interesting upper bound

[TABLE]

on the black-hole resonances in the eikonal $m\gg 1$ limit. This newly derived bound should be valid for generic spherically-symmetric asymptotically flat black-hole spacetimes.

ACKNOWLEDGMENTS

This research is supported by the Carmel Science Foundation. I thank Yael Oren, Arbel M. Ongo and Ayelet B. Lata for stimulating discussions.