# Testing General Relativity’s No-Hair Theorem with X-Ray Observations of Black Holes

###### Abstract

Despite its success in the weak gravity regime, General Relativity (GR) has yet to be verified in the regime of strong gravity. In this paper, we present the results of detailed ray tracing simulations aiming at clarifying if the combined information from X-ray spectroscopy, timing and polarization observations of stellar mass and supermassive black holes can be used to test GR’s no-hair theorem. The latter states that stationary astrophysical black holes are described by the Kerr-family of metrics with the black hole mass and spin being the only free parameters. We use four “non-Kerr metrics”, some phenomenological in nature and others motivated by alternative theories of gravity, and study the observational signatures of deviations from the Kerr metric. Particular attention is given to the case when all the metrics are set to give the same Innermost Stable Circular Orbit (ISCO) in quasi-Boyer Lindquist coordinates. We give a detailed discussion of similarities and differences of the observational signatures predicted for BHs in the Kerr metric and the non-Kerr metrics. We emphasize that even though some regions of the parameter space are nearly degenerate even when combining the information from all observational channels, X-ray observations of very rapidly spinning black holes can be used to exclude large regions of the parameter space of the alternative metrics. Although it proves difficult to distinguish between the Kerr and non-Kerr metrics for some portions of the parameter space, the observations of very rapidly spinning black holes like Cyg X-1 can be used to rule out large regions for several black hole metrics.

###### pacs:

04.25.dg## I Introduction

In the early 1900’s, Albert Einstein proposed his now famous theory of General Relativity. Since its introduction, General Relativity (GR) has been tested extensively in our solar system. GR has passed all tests with remarkable accuracy, including but not limited to the perihelion shift of Mercury, the deflection of light passing near the Sun, and the Shapiro time delay. These tests were extended beyond the solar system with the discovery of the Hulse-Taylor binary pulsar where the decay rate of the orbital period was found to be consistent with the expected decay due to the loss of energy via gravitational waves (see Will (2006) for a review of the subject). However, despite all of these successes, GR has yet to be verified in the strong gravity regime. The most extreme gravitational fields are found near black holes (BHs), and tests of GR near BHs have received considerable attention (see Psaltis (2008) and references therein). Much of this work makes use of the no-hair theorem of GR which states that the only stationary axially symmetric solutions of the Einstein equations are given by the Kerr/Newman family of metrics. In the case of astrophysical BHs with negligible electrical charge, the Kerr solutions are parameterized by the BH’s geometric mass, , and spin, . The tests of this theorem include using stars orbiting Sagittarius , the supermassive BH in the center of the Milky Way galaxy, to measure its angular momentum and quadrupole moment Will (2008). Gravitational wave observations of merging black holes have the potential to test strong-field GR not only in the stationary, but also in the dynamic regime Dreyer et al. (2004). The work presented in this paper makes use of several recently proposed metrics that contain additional terms which violate the no-hair theorem including those of Johannsen and Psaltis (2011a); Glampedakis and Babak (2006); Aliev and Gümrükçüoǧlu (2005); Pani et al. (2011). These metrics are used to quantify the degree to which spectroscopic, polarimetric, and timing X-ray observations can constrain deviations from the Kerr metric.

The spectral X-ray emission from stellar mass BHs can be characterized by a thermal continuum emitted from the accretion disk along with a power law component originating from hotter - yet mostly thermal - plasma, commonly referred to as the corona (e.g. Gilfanov and Merloni, 2014). The power law emission is modeled using the equation where is the photon index Remillard and McClintock (2006). This emission can either travel directly to the observer or return to the accretion disk and lead to scattered and/or reprocessed emission. The reflection component contains the Fe-K line at 6.4 keV and the Compton hump at energies greater than 20 keV. The prominent Fe-K line comes from the reprocessing of photons in the inner accretion disk and receives its characteristic broadened profile due to gravitational redshift, Doppler effects, and relativistic beaming. This profile can then be fit to determine the BH’s spin Fabian et al. (2000); Brenneman (2013); Reynolds and Nowak (2003). The thermal emission, modeled using the prescription developed by Novikov and Thorne (1973) for a geometrically thin, optically thick disk, can also be used to deduce the spin of stellar mass black holes because it allows one to determine the radius of the Innermost Stable Circular Orbit (ISCO) which is a monotonic function of its spin McClintock et al. (2011, 2014). In the case of supermassive black holes, the thermal disk emission falls into the optical/UV bands. As many different emission components contribute to the observed emission in these bands, fitting the Fe-K line is the only way to determine the spin of these systems.

Polarimetric observations with photoelectric effect polarimeters like the ones used on the IXPE, PRAXyS, and XIPE missions currently studied by NASA (IXPE Weisskopf et al. (2014) and PRAXyS Jahoda et al. (2015)) and ESA (XIPE Soffitta et al. (2013)) or with scattering polarimeters such as PolSTAR Beilicke et al. (2012, 2014); Guo et al. (2013) provide a new way to study inner structure of accretion flows. Polarimeters can provide geometrical information even though the inner accretion flow of most black holes are too small to be imaged with the current or even next-generation telescopes (the only exception being the supermassive black holes Sgr A and M 87 which might be imaged with the Event Horizon Telescope Ricarte and Dexter (2015)). In the case of stellar mass black holes, the thermal X-ray emission is expected to exhibit linear polarization with the polarization fraction being a function of the inclination of the inner accretion disk Li et al. (2009); Schnittman and Krolik (2009). The polarization of the Comptonized emission from the corona depends on the scattering processes in the corona itself and off the accretion disk. Several corona geometries have been studied including the lamp-post model where photons are emitted from a point source directly above the black hole itself Dovčiak et al. (2012). Other corona models assume a wedge or spherical corona geometry surrounding the accretion disk (e.g. Schnittman and Krolik, 2010, and references therein).

In the past several years X-ray reverberation has come into its own as a powerful tool to study accreting black holes. Corona emission scattering off the accretion disk reaches the observer with a time delay relative to the direct corona emission. The energy dependence of the time delays can be used to infer details about the structure of the inner accretion flow. For a sample of AGNs, Fe-K vs. continuum lags have been established along with Compton hump vs. continuum lags (see Kara et al. (2015); Uttley et al. (2014) for a review of the subject). These lags can be fit with numerical models to deduce system parameters such as the inclination and lamp-post height in NGC 4151 Cackett et al. (2014) and an extended corona geometry in 1H0707-495 Wilkins and Fabian (2013).

Several authors have used the alternative BH metrics to find observational signatures of non-GR effects. The following types of observations have been studied: (i) fitting of the thermal X-ray emission from stellar mass black holes Bambi and Barausse (2011); Bambi (2012a); Pun et al. (2008); (ii) fitting of the Fe-K line emission from stellar mass and supermassive black holes Bambi (2013a, b); Johannsen and Psaltis (2013); Psaltis and Johannsen (2012); (iii) spectropolarimetric observations of stellar mass black holes Krawczynski (2012); Liu et al. (2015); (iv) observations of Quasi-Periodic Oscillations (QPOs) Johannsen and Psaltis (2011b); Bambi (2012b); Johannsen (2014); (v) X-ray reverberation observations Jiang et al. (2015); (vi) observations of the radiatively inefficient accretion flow around Sgr Broderick et al. (2014). The studies showed that it is very difficult to observationally distinguish between the Kerr space time and the non-Kerr BH space times as long as the BH spin and the parameter describing the deviation from the Kerr space time are free parameters that both need to be derived from the observations.

Several approaches have been discussed to break the degeneracy between the BH spin and deviation parameter(s). In Bambi (2012a, c), for example, it is proposed that the BH spin can be measured independently from the accretion disk properties based on measuring the jet power, although this method faces several difficulties in practice Narayan and McClintock (2012). Furthermore, the observed results depend on the physics of the accretion disk, the radiation transport around the black hole, the physics of launching and accelerating the jet, and the physics of converting the mechanical and electromagnetic jet energy into observable electromagnetic jet emission.

This paper follows up on the work of Krawczynski (2012). The thermal emission from a geometrically thin, optically thick accretion disk is modeled self-consistently for the Kerr metric and the alternative metrics, and observational signatures are derived with the help of a ray-tracing code that tracks photons from their origin to the observer, enabling the modeling of repeated scatterings of the photons off the accretion disk. This paper adds to the previous work by (i) covering the Kerr metric, the metric of Johannsen and Psaltis (2011) Johannsen and Psaltis (2011a) and three additional metrics, (ii) by modeling not only the thermal disk emission but also the emission from a lamp-post corona and the reprocessing of the coronal emission by the accretion disk, and (iii) by considering many observational channels. We analyze the multi-temperature continuum emission from the accretion disk, the energy spectra of the reflected emission (including the Fe K- line and the Compton hump), the orbital periods of matter orbiting the black hole close to the ISCO, the time lags between the Fe K- emission and the direct corona emission, and the size and shape of the black hole shadows.

The rest of the paper is organized as follows. Section 2 begins with a summary of the alternative spacetimes used in this paper and goes on to discuss the model for both the thermal and coronal emission. In Section 3 we compare the observational signatures of the Kerr and the non-Kerr metrics finding that the observational differences are rather small given the uncertainties about the properties of astrophysical accretion disks. We summarize the results in Sect. 4 and emphasize that even though the Kerr and non-Kerr metrics can produce similar observational signatures for some regions of the respective parameter spaces, we can use X-ray observations of black holes from the literature to rule out large regions of the parameter space of the non-Kerr metrics.

Throughout this paper we assume ; all distances are given in units of the gravitational radius, .

## Ii Methodology

### ii.1 Alternative Metrics

As a way to test the no-hair theorem of general relativity, several non-Kerr metrics have been introduced which contain additional parameters apart from the BH’s mass and spin. In this paper we employ the use of four non-GR metrics including two phenomenological metrics Johannsen and Psaltis (2011a); Glampedakis and Babak (2006) and two which are solutions to alternative theories of gravity Aliev and Gümrükçüoǧlu (2005); Pani et al. (2011). All metrics are variations of the Kerr metric in (quasi) Boyer Lindquist coordinates .

The phenomenological metric of Johannsen and Psaltis, 2011 Johannsen and Psaltis (2011a) (JP) reads:

(1) | ||||

with

(2) |

(3) |

The metric was derived by modifying the temporal and radial components of the Schwarzschild line element by a term . The metric does not exhibit any pathologies outside the event horizon and can be used for slowly and rapidly spinning black holes. Asymptotic flatness constrains the leading terms of the expansion of in powers of and the lowest order correction reads:

(4) |

In the limit as this metric reduces to the Kerr solution in Boyer-Lindquist coordinates.

Glampedakis and Babak, 2006 Glampedakis and Babak (2006) (GB) introduced a metric for slowly spinning black holes (). This quasi-Kerr metric in Boyer-Lindquist coordinates is

(5) |

where is the Kerr metric and is given by

(6) | |||||

where and are defined in Appendix A in Glampedakis and Babak (2006). It is clear to see that equation 5 reduces to the Kerr metric when . The details of the JP and GB space times are described in Johannsen (2013a).

Another solution is presented by Aliev and Gümrükçüoǧlu, 2005 Aliev and Gümrükçüoǧlu (2005) describing an axisymmetric, stationary metric for a rapidly rotating black hole which is on a 3-brane in the Randall-Sundrum braneworld. The metric turns out to be identical to GR’s Kerr-Newman metric of an electrically charged spinning black hole, the only difference that is not the electrical charge but a “tidal charge”. The metric (referred to as KN-metric in the following) is given by:

(7) | ||||

with being the same as equation 2 and with .

Pani et al, 2011 Pani et al. (2011) (PMCC) give a family of solutions for slowly rotating BHs derived augmenting the Einstein-Hilbert action by quadratic and algebraic curvature invariants coupling to a single scalar field. The action is given by the expression:

(8) | ||||

where

(9) |

for , is the matter action containing a generic non-minimal coupling, and is the scalar self potential. When the metric reduces to the one for Chern-Simons gravity and when it becomes the Gauss-Bonnet solution.

### ii.2 Thermal Accretion Disk Emission and Photon Propagation

The code models the emission of photons and their propagation self-consistently for the Kerr and non-Kerr metrics Krawczynski (2012). The radial emission profile of the geometrically thin, optically thick accretion disk is calculated based on the general solution of Novikov and Thorne Novikov and Thorne (1973), the relativistic extension of the Shakura-Sunyaev equations Shakura and Sunyaev (1973). Writing the considered Kerr or non-Kerr metric in the form

(10) |

the conservation of rest mass, angular momentum, and energy give the following disk brightness in the rest frame of the emitting plasma Page and Thorne (1974):

(11) |

with

(12) |

Here, is the time averaged rate of accretion. The solution assumes a vanishing torque at the ISCO. We calculate the by finding the location where the energy is a minimum by solving the equation for planar, circular orbits.

We model photons emitted between and 100 that are tracked until they either fall into black hole or reach a coordinate stationary observer at 10,000 . The photon trajectories are calculated by integrating the geodesic equations:

(13) |

with a fourth order Runge Kutta method. The ’s are the Christoffel symbols and is the affine parameter. Tracking photons forward in time makes it possible to model trajectories with multiple scattering events and/or with the absorption and re-emission of photons in the accretion disk and/or in the corona. The initial polarization and the change in polarization upon scattering are calculated with the help of Chandrasekhar’s results for optically thick atmospheres Chandrasekhar (1960). The polarization vector, f is parallel transported according to the following equation

(14) |

A more detailed description of the code can be found in Krawczynski (2012).

### ii.3 Lamp-Post Corona Model

We utilize the commonly used lamp-post model (e.g. Matt et al., 1991; Dovciak, 2004) to simulate the coronal power-law emission. Unpolarized 1-100 keV photons are emitted from a point source above the black hole. The height of the point source can be constrained based on fitting the Fe-K vs. continuum emission lag (e.g. Cackett et al., 2014). Alternatively, the corona may be associated with a region of energy dissipation close to the base of a jet. The trajectory of the photons and their change in polarization upon scattering off the accretion disk are calculated as described above. Photons impinging on the accretion disk can either be absorbed, prompt the emission of a Fe-K fluorescence photon, or Compton scatter. A diagram of the various types of emission modeled can be seen in Fig. 1.

The results of George and Fabian (1991) were used to determine the probability of the creation of the Fe-K photons and Compton reflections. The results can then be analyzed to examine the time lag between the direct power-law emission and the Fe-K emission from 2-10 keV following the methodology described in Cackett et al. (2014). We analyze the Fourier transform of the transfer function to infer the time lag as a function of Fourier frequency.

## Iii Results

Previous analyses have shown that the Kerr and non-Kerr metrics give similar spectral and spectropolarimetric signatures if the parameters are chosen to give the same (e.g. Krawczynski, 2012; Bambi, 2013a; Jiang et al., 2015; Johannsen, 2014; Johannsen and Psaltis, 2013; Kong et al., 2014). Figure 2

shows as a function of the BH spin and the parameter characterizing the deviation from the Kerr metric for the JP and KN metrics. We see that for all JP and KN metrics, we can always find one and only one Kerr metric with the same . The mapping is not unambiguous the other way around: the JP and KN metrics can give one for several different combinations of the BH spin and the deviation parameter.

In the following we focus on comparing “degenerate” models which give the same . We consider a slowly spinning Kerr black hole () and a rapidly spinning Kerr black hole () and JP and KN models giving the same (see Table 1).

Metric | Spin | Deviation | (g/s) | |
---|---|---|---|---|

Kerr | 0.9 | none | 2.32 | 8.98 |

JP | 0.5 | 6.33 | 2.32 | 7.51 |

KN | 0.5 | 0.69 | 2.32 | 9.86 |

Kerr | 0.2 | none | 5.33 | 2.16 |

GB | 0.25 | 5.33 | 2.15 | |

PMCC | 0.29 | , | 5.33 | 2.11 |

In the following we show the Kerr, GB and PMCC results for the low-spin case, and the Kerr, KN and JP results for the high-spin case. We adjusted the accretion rates to give the same accretion luminosity (extracted gravitational energy per unit observer time) for all considered metrics. This is done by normalizing the accretion rate by the efficiency which is not corrected for the fraction of photons escaping to infinity.

The left panels of Figs. 3 and 4 compare the fluxes emitted in the plasma frame for the different metrics. For the rapidly spinning black holes (Fig. 2(a)), the fractional differences in are typically a few percent. The difference is larger for the innermost part of the accretion flow with the Kerr exceeding the values of the non-Kerr metrics by up to 30%.

The right panels of the figures show the power emitted per unit Boyer Lindquist time and per Boyer Lindquist radial interval :

(15) |

The factor is the dependent part of the metric and is used to transform the number of emitted photons per plasma frame and into that emitted per Boyer Lindquist and Kulkarni et al. (2011). The last factor corrects for the frequency change of the photons between their emission in the plasma rest frame and their detection by an observer at infinity. We estimate the effective redshift between emission and observation by assuming photons are emitted in the upper hemisphere with the dimensionless wave vector in the plasma frame. After transforming into the wave vector in the Boyer Lindquist frame we calculate the photon energy at infinity from the constant of motion associated with the time translation Killing vector :

(16) |

and set . The different metrics exhibit very similar -distributions with typical fractional differences of 10%. Again, the largest deviations are found near the ISCO. Overall, the different metrics lead to very similar and -distributions because (i) we compare models with identical -values (leading radial profiles with a similar -dependence), and (ii) we use fine-tuned accretion rates to compensate for the different accretion efficiencies where (i.e. the different fractions of the rest mass energy that can be extracted when matter moves from infinity to ). In the following we focus on the rapidly spinning BH simulations, as the observables depend more strongly on the assumed background spacetime than for slowly spinning BHs.

The analysis presented here focuses on specific choices for matching the Kerr metric with non-Kerr counterparts. This matching is not unique as the non-Kerr metrics give the same for a continuous family of different metrics. We simulated a few non-Kerr metrics giving the same , and found that the differences between these metrics and the Kerr metric are all comparable to the differences shown above.

Figure 5 shows the flux, polarization degree, and polarization direction of the thermal disk emission of a mass accreting stellar mass BH as shown for an observer at an inclination of 75.We only show the results for the rapidly spinning Kerr, JP and KN BHs. While there are some differences in these spectra the overall shapes are similar. At the highest energies, deep in the Wien tail of the multi-temperature energy spectrum, the fluxes show more differences owing to the different orbital velocities and thus Doppler boost of the emission and different fractions of photons reaching the observer versus photons falling into the BHs. The different metrics also lead to very similar polarization fractions and polarization angles. However, in terms of the polarization properties the Kerr and KN metrics show almost identical results and the JP metric shows slightly different results. Overall, the main conclusion is that once we choose models with identical and correct for the different accretion efficiencies, the observational signatures depend only very weakly on the considered metric. Assuming that the background spacetime is described by the Kerr metric, the thermal energy spectrum and the polarization properties can be used to fit and the BH inclination Li et al. (2009); Schnittman and Krolik (2009). The results presented so far indicate that the fitted and values will not depend strongly on the assumed background spacetime.

We now turn to the properties of the reflected corona emission from an AGN, assuming the lamp-post corona emits unpolarized emission with a photon power law index of 1.7 from a height 3 above the black hole (Fig. 6). Again, the flux and polarization energy spectra are almost the same for all considered metrics. The KN metric shows slightly larger deviations from the Kerr metric than the JP metric.

Some accreting black holes exhibit quasi periodic oscillations (QPOs), i.e. peaks in the Fourier transformed power spectra. The orbiting hot spot model Schnittman and Bertschinger (2004); Schnittman (2005); Stella and Vietri (1998, 1999); Abramowicz and Kluźniak (2001, 2003) explains the high-frequency QPOs (HFQPOs) of accreting stellar mass black holes with a hot spot orbiting the black hole close to the ISCO. If we succeeded to confirm the model (e.g. through the observations of the phase resolved energy spectra and/or polarization properties Behestipour et al. (2015)), one could use HFQPO observations to measure the orbital periods close to the ISCO. In the case of AGNs, tentative evidence for periodicity associated with the ISCO has been found for several objects. Examples include orbital periodicity on the time scale of a few days as seen in the blazar OJ 287 Pihajoki et al. (2013) and QPO’s at frequencies of O(100 Hz) such as that seen for the microquasar GRO J1655-40 Strohmayer (2001).

Figure 7 shows that different metrics do predict different orbital periods which vary by up to 10%.

We investigated if other timing properties can be used to observationally distinguish between the different metrics by analyzing the observable time lags between the direct corona emission and the reflected emission assuming the lamp post geometry. We use the standard X-ray reverberation analysis methods described by Uttley et al. (2014). As expected, the 2-10 keV flux variations lag the 1-2 keV flux variations (Figure 8). The JP metric leads to time lags up to 24% shorter than the Kerr and KN metrics at low frequencies. At frequencies between 0.01 and 0.1 phase wrapping begins to occur (when the lag changes sign and begins to oscillate around 0) leading to the larger differences seen in this range.

Although the considered metrics give the same in Boyer-Lindquist coordinates, the black hole shadow may have a different shape and/or size when viewed by an observer at infinity (see Johannsen and Psaltis, 2010; Johannsen, 2013b, for a related study). The results for the Kerr, JP, and KN metrics are shown in Fig. 9

for an inclination of . The shadow of the KN and JP metrics is 15% smaller than that of the Kerr metric. Furthermore, the shapes differ slightly. Similarly, the shapes of the photon rings are shown in Fig. 10 which are calculated by following the procedures outlined in Section III of Bardeen (1973).

## Iv Summary and Discussion

In this paper we studied the observational differences between accreting black holes in five different background spacetimes, including GR’s Kerr spacetime, and four alternative spacetimes. We chose the parameters of the considered metrics as to give identical innermost stable orbits in Boyer Lindquist coordinates. The predicted observational differences are larger for rapidly spinning black holes. Overall the observational differences are very small if we adjust the accretion rate to correct for the metric-dependent accretion efficiency. The measurement of the predicted differences are very small – especially if one accounts for the astrophysical uncertainties, i.e. observational and theoretical uncertainties of the accretion disk properties. From an academic standpoint, it is interesting to compare the small differences of the predicted properties, e.g. the differences of the thermal energy spectra and the BH shadow images. The thermal spectrum of the Kerr BH is slightly harder than that of the JP and KN black holes (for the same ), and the Kerr BH shadow is slightly larger than that the JP and KN BH shadows. Reducing the spin of the Kerr BH would make the spectral difference smaller, but would increase the mismatch between the apparent BH shadow diameters. Thus, in the absence of astrophysical uncertainties, the combined information from various observational channels could be used to distinguish between different metrics.

Although the analysis shows that the differences between the Kerr and non-Kerr metrics are rather subtle (especially in the presence of uncertainties of the structure of astrophysical accretion disks), we can use existing observations to constrain large parts of the parameter space of the non-Kerr metrics (see also Bambi (2014)). As an example we use the recent observations of the accreting stellar mass black hole Cyg X-1 Gou et al. (2011). The observations give a 3 upper limit of . Inspecting Fig.2 we see that the constraints on the ISCO can only be fulfilled for JP deviation parameters and KN deviation parameters , excluding all parameter values outside of these intervals. Our limits rest on the matching of Kerr to non-Kerr metrics via using identical -values. Maximally rotating black holes, when a 0.998 Thorne (1974) provide the best opportunity to test GR because observations of these systems can, in principle, be used to exclude all deviations from GR down to a small interval around 0, limited only by the actual spin value, the statistics of the observations, and the astrophysical uncertainties. A follow-up analysis could use state-of-the-art modeling of the actual X-ray data with accretion disk and emission models in the Kerr and non-Kerr background spacetimes.

Further progress will be achieved by continuing to refine our understanding of BH accretion disks based on General Relativistic Magnetohydrodynamic and General Relativistic Radiation Magnetohydrodynamic simulations (e.g. Schnittman and Krolik, 2013; Schnittman et al., 2013; Sadowski and Narayan, 2015) and matching simulated observations to X-ray spectroscopic, X-ray polarization, and X-ray reverberation observations.

The images of the BH shadow of Sgr A with the Event Horizon Telescope can give additional constraints. Whereas the images of the BH shadow still depend on the astrophysics of the accretion disk, imaging of the photon ring would be free of such uncertainties. Of course, much better imaging would be required to do so.

###### Acknowledgements.

We would like to thank NASA (grant #NNX14AD19G) and the Washington University McDonnell Center for the Space Sciences for financial support.## References

- Will (2006) C. M. Will, Living Reviews in Relativity 9, 3 (2006).
- Psaltis (2008) D. Psaltis, Living Reviews in Relativity 11, 9 (2008).
- Will (2008) C. M. Will, ApJL 674, L25 (2008).
- Dreyer et al. (2004) O. Dreyer, B. Kelly, B. Krishnan, L. S. Finn, D. Garrison, and R. Lopez-Aleman, Classical and Quantum Gravity 21, 787 (2004).
- Johannsen and Psaltis (2011a) T. Johannsen and D. Psaltis, PRD 83, 124015 (2011a).
- Glampedakis and Babak (2006) K. Glampedakis and S. Babak, Classical and Quantum Gravity 23, 4167 (2006).
- Aliev and Gümrükçüoǧlu (2005) A. N. Aliev and A. E. Gümrükçüoǧlu, PRD 71, 104027 (2005).
- Pani et al. (2011) P. Pani, C. F. B. Macedo, L. C. B. Crispino, and V. Cardoso, PRD 84, 087501 (2011).
- Gilfanov and Merloni (2014) M. Gilfanov and A. Merloni, SSR 183, 121 (2014).
- Remillard and McClintock (2006) R. A. Remillard and J. E. McClintock, ARAA 44, 49 (2006).
- Fabian et al. (2000) A. C. Fabian, K. Iwasawa, C. S. Reynolds, and A. J. Young, PASP 112, 1145 (2000).
- Brenneman (2013) L. Brenneman, Measuring the Angular Momentum of Supermassive Black Holes, SpringerBriefs in Astronomy. ISBN 978-1-4614-7770-9. Laura Brenneman, 2013 (2013).
- Reynolds and Nowak (2003) C. S. Reynolds and M. A. Nowak, Phys. Rep. 377, 389 (2003).
- Novikov and Thorne (1973) I. D. Novikov and K. S. Thorne, in Black Holes (Les Astres Occlus), edited by C. Dewitt and B. S. Dewitt (1973) pp. 343–450.
- McClintock et al. (2011) J. E. McClintock, R. Narayan, S. W. Davis, L. Gou, A. Kulkarni, J. A. Orosz, R. F. Penna, R. A. Remillard, and J. F. Steiner, Classical and Quantum Gravity 28, 114009 (2011).
- McClintock et al. (2014) J. E. McClintock, R. Narayan, and J. F. Steiner, Space Sci Rev 183, 295 (2014).
- Weisskopf et al. (2014) M. C. Weisskopf, R. Bellazzini, E. Costa, G. Matt, H. L. Marshall, S. L. O’Dell, G. G. Pavlov, B. Ramsey, and R. W. Romani, in AAS/High Energy Astrophysics Division, AAS/High Energy Astrophysics Division, Vol. 14 (2014) p. 116.15.
- Jahoda et al. (2015) K. Jahoda, C. Kouveliotou, T. R. Kallman, and Praxys Team, in American Astronomical Society Meeting Abstracts, American Astronomical Society Meeting Abstracts, Vol. 225 (2015) p. 338.40.
- Soffitta et al. (2013) P. Soffitta, X. Barcons, R. Bellazzini, J. Braga, E. Costa, G. W. Fraser, S. Gburek, J. Huovelin, G. Matt, M. Pearce, J. Poutanen, V. Reglero, A. Santangelo, R. A. Sunyaev, G. Tagliaferri, and others, Experimental Astronomy 36, 523 (2013).
- Beilicke et al. (2012) M. Beilicke, M. G. Baring, S. Barthelmy, W. R. Binns, J. Buckley, R. Cowsik, P. Dowkontt, Q. Guo, Y. Haba, M. H. Israel, H. Kunieda, K. Lee, J. Martin, H. Matsumoto, T. Miyazawa, T. Okajima, J. Schnittman, K. Tamura, J. Tueller, and H. Krawczynski, in American Institute of Physics Conference Series, American Institute of Physics Conference Series, Vol. 1505, edited by F. A. Aharonian, W. Hofmann, and F. M. Rieger (2012) pp. 805–808.
- Beilicke et al. (2014) M. Beilicke, F. Kislat, A. Zajczyk, Q. Guo, R. Endsley, M. Stork, R. Cowsik, P. Dowkontt, S. Barthelmy, T. Hams, T. Okajima, M. Sasaki, B. Zeiger, G. de Geronimo, M. G. Baring, and H. Krawczynski, Journal of Astronomical Instrumentation 3, 1440008 (2014).
- Guo et al. (2013) Q. Guo, M. Beilicke, A. Garson, F. Kislat, D. Fleming, and H. Krawczynski, Astroparticle Physics 41, 63 (2013).
- Ricarte and Dexter (2015) A. Ricarte and J. Dexter, MNRAS 446, 1973 (2015).
- Li et al. (2009) L.-X. Li, R. Narayan, and J. E. McClintock, ApJ 691, 847 (2009).
- Schnittman and Krolik (2009) J. D. Schnittman and J. H. Krolik, ApJ 701, 1175 (2009).
- Dovčiak et al. (2012) M. Dovčiak, F. Muleri, R. W. Goosmann, V. Karas, and G. Matt, Journal of Physics Conference Series 372, 012056 (2012).
- Schnittman and Krolik (2010) J. D. Schnittman and J. H. Krolik, ApJ 712, 908 (2010).
- Kara et al. (2015) E. Kara, A. Zoghbi, A. Marinucci, D. J. Walton, A. C. Fabian, G. Risaliti, S. E. Boggs, F. E. Christensen, F. Fuerst, C. J. Hailey, F. A. Harrison, G. Matt, M. L. Parker, C. S. Reynolds, D. Stern, and W. W. Zhang, MNRAS 446, 737 (2015).
- Uttley et al. (2014) P. Uttley, E. M. Cackett, A. C. Fabian, E. Kara, and D. R. Wilkins, A&ARev 22, 72 (2014).
- Cackett et al. (2014) E. M. Cackett, A. Zoghbi, C. Reynolds, A. C. Fabian, E. Kara, P. Uttley, and D. R. Wilkins, MNRAS 438, 2980 (2014).
- Wilkins and Fabian (2013) D. R. Wilkins and A. C. Fabian, MNRAS 430, 247 (2013).
- Bambi and Barausse (2011) C. Bambi and E. Barausse, ApJ 731, 121 (2011).
- Bambi (2012a) C. Bambi, PRD 85, 043002 (2012a).
- Pun et al. (2008) C. S. J. Pun, Z. Kovács, and T. Harko, PRD 78, 084015 (2008).
- Bambi (2013a) C. Bambi, PRD 87, 023007 (2013a).
- Bambi (2013b) C. Bambi, JCAP 8, 55 (2013b).
- Johannsen and Psaltis (2013) T. Johannsen and D. Psaltis, ApJ 773, 57 (2013).
- Psaltis and Johannsen (2012) D. Psaltis and T. Johannsen, ApJ 745, 1 (2012).
- Krawczynski (2012) H. Krawczynski, ApJ 754, 133 (2012).
- Liu et al. (2015) D. Liu, Z. Li, Y. Cheng, and C. Bambi, European Physical Journal C 75, 383 (2015).
- Johannsen and Psaltis (2011b) T. Johannsen and D. Psaltis, ApJ 726, 11 (2011b).
- Bambi (2012b) C. Bambi, JCAP 9, 14 (2012b).
- Johannsen (2014) T. Johannsen, PRD 90, 064002 (2014).
- Jiang et al. (2015) J. Jiang, C. Bambi, and J. F. Steiner, JCAP 5, 025 (2015).
- Broderick et al. (2014) A. E. Broderick, T. Johannsen, A. Loeb, and D. Psaltis, ApJ 784, 7 (2014).
- Bambi (2012c) C. Bambi, PRD 85, 043001 (2012c).
- Narayan and McClintock (2012) R. Narayan and J. E. McClintock, MNRAS 419, L69 (2012).
- Johannsen (2013a) T. Johannsen, PRD 87, 124017 (2013a).
- Shakura and Sunyaev (1973) N. I. Shakura and R. A. Sunyaev, AAP 24, 337 (1973).
- Page and Thorne (1974) D. N. Page and K. S. Thorne, ApJ 191, 499 (1974).
- Chandrasekhar (1960) S. Chandrasekhar, Radiative transfer (New York: Dover, 1960).
- Matt et al. (1991) G. Matt, G. C. Perola, and L. Piro, A&A 247, 25 (1991).
- Dovciak (2004) M. Dovciak, Ph.D. thesis, http://adsabs.harvard.edu/abs/2004PhDT…….331D (2004).
- George and Fabian (1991) I. M. George and A. C. Fabian, MNRAS 249, 352 (1991).
- Kong et al. (2014) L. Kong, Z. Li, and C. Bambi, ApJ 797, 78 (2014).
- Kulkarni et al. (2011) A. K. Kulkarni, R. F. Penna, R. V. Shcherbakov, J. F. Steiner, R. Narayan, A. Sädowski, Y. Zhu, J. E. McClintock, S. W. Davis, and J. C. McKinney, MNRAS 414, 1183 (2011).
- Schnittman and Bertschinger (2004) J. D. Schnittman and E. Bertschinger, ApJ 606, 1098 (2004).
- Schnittman (2005) J. D. Schnittman, ApJ 621, 940 (2005).
- Stella and Vietri (1998) L. Stella and M. Vietri, ApJL 492, L59 (1998).
- Stella and Vietri (1999) L. Stella and M. Vietri, Physical Review Letters 82, 17 (1999).
- Abramowicz and Kluźniak (2001) M. A. Abramowicz and W. Kluźniak, AAP 374, L19 (2001).
- Abramowicz and Kluźniak (2003) M. A. Abramowicz and W. Kluźniak, General Relativity and Gravitation 35, 69 (2003).
- Behestipour et al. (2015) B. Behestipour, J. K. Hoormann, and H. Krawczynski, submitted to ApJ (2015).
- Pihajoki et al. (2013) P. Pihajoki, M. Valtonen, and S. Ciprini, MNRAS 434, 3122 (2013).
- Strohmayer (2001) T. E. Strohmayer, ApJL 552, L49 (2001).
- Johannsen and Psaltis (2010) T. Johannsen and D. Psaltis, ApJ 718, 446 (2010).
- Johannsen (2013b) T. Johannsen, ApJ 777, 170 (2013b).
- Bardeen (1973) J. M. Bardeen, in Black Holes (Les Astres Occlus), edited by C. Dewitt and B. S. Dewitt (1973) pp. 215–239.
- Bambi (2014) C. Bambi, Physics Letters B 730, 59 (2014).
- Gou et al. (2011) L. Gou, J. E. McClintock, M. J. Reid, J. A. Orosz, J. F. Steiner, R. Narayan, J. Xiang, R. A. Remillard, K. A. Arnaud, and S. W. Davis, ApJ 742, 85 (2011).
- Thorne (1974) K. S. Thorne, ApJ 191, 507 (1974).
- Schnittman and Krolik (2013) J. D. Schnittman and J. H. Krolik, ApJ 777, 11 (2013).
- Schnittman et al. (2013) J. D. Schnittman, J. H. Krolik, and S. C. Noble, ApJ 769, 156 (2013).
- Sadowski and Narayan (2015) A. Sadowski and R. Narayan, ArXiv e-prints (2015), arXiv:1508.04980 .