• Corpus ID: 231582913

Gravitational wave templates from Extreme Mass Ratio Inspirals

@inproceedings{Skoupy2021GravitationalWT,
  title={Gravitational wave templates from Extreme Mass Ratio Inspirals},
  author={Viktor Skoup'y and Georgios Lukes-Gerakopoulos Institute of Theoretical Physics and Faculty of Mathematics and Physics and Charles University and Prague and Czech Republic and Astronomical Institute of the Slovak Academy of Sciences},
  year={2021}
}

• Viktor Skoup'y, Georgios Lukes-Gerakopoulos Institute of Theoretical Physics, +5 authors A. Sciences
• Published 12 January 2021
• Physics

An extreme mass ratio inspiral takes place when a compact stellar object is inspiraling into a supermassive black hole due to gravitational radiation reaction. Gravitational waves (GWs) from this system can be calculated using the Teukolsky equation (TE). In our case, we compute the asymptotic GW fluxes of a spinning body orbiting a Kerr black hole by solving numerically the TE both in time and frequency domain. Our ultimate goal is to produce GW templates for space-based detectors such as LISA. Introduction The Laser Interferometer Space Antenna (LISA) is a future space based gravitational wave (GW) detector planned to launch in 2030s [Amaro-Seoane et al., 2017]. LISA will consist of three spacecrafts forming an equilateral triangle with sides 2.5 million km long on heliocentric orbit. Changes in the distance between the spacecrafts will be monitored by Michelson-like interferometers with high precision. When a GW passes this constellation, the spacetime between the spacecrafts will be quasi-periodically stretched and contracted in the direction perpendicular to the propagation of the wave. Hence, LISA will be able to detect the wave, including its amplitude and phase, by measuring the changes in the distance between the three spacecrafts. This GW observatory will be sensitive in frequencies around 10−3 Hz. One type of events LISA will be able to detect are extreme mass ratio inspirals (EMRIs). It is expected that the centre of galaxies host supermassive black holes with masses in the range of 106–109M . An EMRI takes place when a stellar mass black hole or a neutron star is inspiraling into a supermassive black hole while losing energy and angular momentum due to gravitational radiation reaction. Such a system is emitting GWs that should be detectable far away from the source in the mHz bandwidth. A GW signal from an EMRI can provide important information about the parameters of the system such as the masses of the objects, their spins etc. Actually EMRIs’ detection will give us the opportunity to map the spacetime around a supermassive black hole to high accuracy. Since the parameter analysis of the detected GW signal depends on the accuracy of the waveform templates, it is important to model an EMRI with adequate precision and find theoretical waveforms from EMRI systems for various parameters. The radiation reaction that acts on a moving particle can be split in two parts: a dissipative and a conservative one. In this work, we focus on the dissipative part, which can be calculated from the energy and angular momentum fluxes at the horizon of the black hole and at infinity. To obtain the leading term in the evolution of the GW phase, it is sufficient to consider only time averages of the dissipative part [Barack and Pound, 2019]. This approximation is called adiabatic. In this case, the particle is slowly shifted from one orbit to another on time scale much larger than the orbital period. In this paper, we first review the properties of a spinning test particle moving in the Kerr ar X iv :2 10 1. 04 53 3v 1 [ gr -q c] 1 2 Ja n 20 21 SKOUPY AND LUKES-GERAKOPOULOS: GW TEMPLATES FROM EMRI spacetime. Then we summarize the Teukolsky formalism, which allows us to calculate the energy and angular momentum fluxes along with the waveforms. Using this formalism we calculate the energy fluxes from circular equatorial orbits of spinning particles around Schwarzschild and Kerr black holes. Subsequently, we use these fluxes to adiabatically evolve circular equatorial orbits and to find the effects of spin of the secondary object on the GW phase. Throughout the paper, we use geometrical units G = c = 1, where G is the gravitational constant and c is the speed of light, and the metric signature (−+++). Spinning test particles in the Kerr geometry The Kerr geometry, which describes a rotating black hole in vacuum, is represented in Boyer-Lindquist coordinates (t, r, θ, φ) by the metric [Misner et al., 2017] ds = − Σ ( dt− a sin θdφ )2 + Σ ∆ dr + Σdθ + sin θ Σ (( r + a ) dφ− adt )2 (1) where ∆ = r − 2Mr + a , Σ = r + a cos θ . (2) This metric depends on two parameters: the mass of the black hole M and the Kerr parameter a. The internal angular momentum (spin) of a Kerr black hole is aM . At the radius r+ = M + √ M2 − a2, where ∆ = 0, the outer event horizon is located. In this paper, we are dealing only with the region r > r+. For a = 0 the Kerr spacetime reduces to the Schwarzschild one. A compact test object in general relativity can be characterized just by its multipoles [Dixon, 1964]. For example, a rotating black hole or a neutron star moving in a Kerr background can be modeled using a pole-dipole approximation, where only the mass and the spin of these compact objects are taken into account, reducing them to a spinning test particle. The poledipole approximation holds as long as the size of the test body is smaller than the scale of the background curvature. The stress-energy tensor of a spinning test particle reads [Ehlers, 1979] T = 1 √ −g ( v(μpν) v0 δ −∇α ( Sα(μvν) v0 δ )) (3) where g is the determinant of the metric, vμ = dxμ dτ is the four-velocity, pμ is the four-momentum, Sμν is the spin tensor, δ3 = δ(r − rp(t))δ(θ − θp(t))δ(φ − φp(t)) where rt(t), θp(t) and φp(t) are the coordinates of the particle depending at the coordinate time t. The conservation of the stress-energy tensor (3) leads to the Mathisson-Papapetrou-Dixon (MPD) equations [Mathisson, 1937; Papapetrou, 1951; Dixon, 1964] Dpμ dτ = − 2 Rνκλv S , (4) DSμν dτ = pv − pv , (5) where τ is the proper time and Rνκλ is the Riemann tensor. The centre of mass for an extended body in general relativity is not uniquely defined. To fix the centre of mass for a spinning body, one has to specify the so called spin-supplementary condition (SSC). In this work we use the Tulczyjew-Dixon SSC [Dixon, 1964], which reads Spμ = 0 . (6) and closes the MPD system. Actually, this SSC allows an explicit relation of the dependence of the four-velocity vμ on the four-momentum pμ [Ehlers and Rudolph, 1977]. SKOUPY AND LUKES-GERAKOPOULOS: GW TEMPLATES FROM EMRI The magnitude of the spin is defined as S2 = SSμν/2, while the mass of the particle is μ2 = −ppμ. Both of these quantities are conserved under Tulczyjew-Dixon SSC. Instead of the measure of the spin S, its dimensionless counterpart σ = S/(μM) is often used in EMRI studies. For this dimensionless spin holds σ ' μ/M ≡ q, i.e. it is of the order of an EMRI mass ratio. There are two Killing vectors in the Kerr geometry ξ (t) = ∂xμ ∂t , ξ (φ) = ∂xμ ∂φ , (7) providing respectively two conserved quantities for the spinning particle E = −ξ (t)pμ + 1 2 ξ μ;νS μν , (8) Jz = ξ μ (φ)pμ − 1 2 ξ μ;νS μν . (9) These quantities can be interpreted at infinity as the energy and the component of the total angular momentum parallel to the rotational axis of the central black hole (z-axis). Teukolsky equation The mass ratio q of an EMRI lies between 10−7 and 10−4. Thanks to this, the GWs from such systems have relatively low amplitudes and perturbation theory can be employed. Using Newman-Penrose formalism it is possible to find equations governing the perturbation of the Weyl tensor projected on some tetrad. Teukolsky [1973] found the master equation (Teukolsky equation, TE) (( r2 + a2 )2 ∆ − a sin θ ) ∂2ψ ∂t2 + 4Mar ∆ ∂2ψ ∂t∂φ + ( a2 ∆ − 1 sin θ ) ∂2ψ ∂φ2 −∆−s ∂ ∂r ( ∆ ∂ψ ∂r ) − 1 sin θ ∂ ∂θ ( sin θ ∂ψ ∂θ ) − 2s ( a(r −M) ∆ + i cos θ sin θ ) ∂ψ ∂φ − 2s ( M ( r2 − a2 ) ∆ − r − ia cos θ ) ∂ψ ∂t + ( s cot θ − s ) ψ = 4πΣT , (10) which governs scalar, neutrino, electromagnetic and gravitational perturbations of the Kerr spacetime. s denotes the spin weight of the field and ψ is a projection of the field quantity on a tetrad depended on s, while T is the source term. For GWs at infinity it is useful to calculate the quantity Ψ4 = ρ 4ψ for s = −2, where ρ = −1/(r − ia cos θ). Then the source term consists of derivatives of the stress-energy tensor projected on the tetrad. This equation is usually decomposed into azimuthal m-modes