Abstract
This work focuses on some key aspects of the general relativistic (GR)—magneto-hydrodynamic (MHD) applications in high-energy astrophysics. We discuss the relevance of the GRHD counterparts formulation exploring the geometrically thick disk models and constraints of the GRMHD shaping the physics of accreting configurations. Models of clusters of tori orbiting a central super-massive black hole (SMBH) are described. These orbiting tori aggregates form sets of geometrically thick, pressure supported, perfect fluid tori, associated to complex instability processes including tori collision emergence and empowering a wide range of activities related expectantly to the embedding matter environment of Active Galaxy Nuclei. Some notes are included on aggregates combined with proto-jets, represented by open cusped solutions associated to the geometrically thick tori. This exploration of some key concepts of the GRMHD formulation in its applications to High-Energy Astrophysics starts with the discussion of the initial data problem for a most general Einstein–Euler–Maxwell system addressing the problem with a relativistic geometric background. The system is then set in quasi linear hyperbolic form, and the reduction procedure is argumented. Then, considerations follow on the analysis of the stability problem for self-gravitating systems with determined symmetries considering the perturbations also of the geometry part on the quasi linear hyperbolic onset. Thus we focus on the ideal GRMHD and self-gravitating plasma ball. We conclude with the models of geometrically thick GRHD disks gravitating around a Kerr SMBH in their GRHD formulation and including in the force balance equation of the disks the influence of a toroidal magnetic field, determining its impact in tori topology and stability.
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Notes
We adopt the geometrical units \(c=1=G\) and the \((-,+,+,+)\) signature, Latin indices run in \(\{0,1,2,3\}\). The four-velocity satisfy \(U^a U_a=-1\). The radius r has unit of mass [M], and the angular momentum units of \([M]^2\), the velocities \([U^t]=[U^r]=1\) and \([U^{\phi }]=[U^{\theta }]=[M]^{-1}\) with \([U^{\phi }/U^{t}]=[M]^{-1}\) and \([U_{\phi }/U_{t}]=[M]\). For the seek of convenience, we always consider the dimensionless energy and effective potential \([V_{eff}]=1\) and an angular momentum per unit of mass \([L]/[M]=[M]\).
This also includes effects related to the disks energetics such as the mass-flux, the enthalpy-flux (evaluating also the temperature parameter), and the flux thickness. We assume polytropic fluids with pressure \(p=\kappa \rho ^{1+1/n}\). The mass-flux, enthalpy-flux and flux thickness have all form \({\mathscr {O}}(r_\times ,r_s,n)=q(n,\kappa )(W_s-W_{\times })^{d(n)}\), where \(q(n,\kappa )\) and d(n) are different functions of the polytropic index and constant: \(W_s\ge W_{\times }\) is the value of the equipotential surface, which is taken with respect to the asymptotic value, while \( W_{\times }\) is evaluated at the cusp \(r_{\times }\). Thus there is more specifically \(\mathrm {{{Enthalpy-flux}}}={\mathscr {D}}(n,\kappa ) (W_s-W)^{n+3/2}\), \(\mathrm {{{Mass-Flux}}}= {\mathscr {C}}(n,\kappa ) (W_s-W)^{n+1/2}\). The quantity \({\mathscr {L}}_{\times }/{\mathscr {L}}= {\mathscr {B}}/{\mathscr {A}} (W_s-W_{\times })/(\eta c^2)\) evaluates the fraction of energy produced inside the flow and not radiated through the surface (swallowed by the BH), \(({\mathscr {A}}, {\mathscr {B}},{\mathscr {C}})\) are constant depending on the polytropics. The efficiency is \(\eta \equiv {\mathscr {L}}/{\dot{M}}c^2\), \({\mathscr {L}}\) representing the total luminosity, the \({\dot{M}}\) is the total accretion rate where for a stationary flow \({\dot{M}}={\dot{M}}_\times \) that is the mass flow rate through the cusp (mass loss, accretion rates). Then \({\dot{M}}_\times \), the cusp luminosity \({\mathscr {L}}_\times \) (and the accretion efficiency \(\eta \)), measuring the rate the thermal-energy is carried at cusp, have the compact form \({\mathscr {P}}={\mathscr {O}}(r_\times ,r_s,n) r_\times (\varOmega _K(r_\times ))^{-1}\), where the relativistic frequency \(\varOmega \) reduces to the Keplerian one \(\varOmega _K\) at the edges of the accretion torus because the pressure forces vanish. There is \({\mathscr {L}}_{\times }={{\mathscr {B}}(n,\kappa ) r_{\times } (W_s-W_{\times })^{n+2}}/{\varOmega _K(r_{\times })}\), and accretion rate for the disk is \({\dot{m}}= {\dot{M}}/{\dot{M}}_{Edd}\), while \({\dot{M}}_{\times }={{\mathscr {A}}(n,\kappa ) r_{\times } (W_s-W_{\times })^{n+1}}/{\varOmega _K(r_{\times })}\) [13, 16, 77].
The global non-axis-symmetric hydrodynamic (HD) PPI implies also the formation of long-lasting, large-scale structures that may be also tracer for such tori in the in the gravitational wave emission—see for example [86].
For example in [69], using three-dimensional GRMHD simulations it is studied the interaction between the PPI and the MRI considering an analytical magnetized equilibrium solution as initial condition. In the HD tori, the PPI selects the large-scale \(m = 1\) azimuthal mode as the fastest growing and non-linearly dominant mode. In different works it is practically shown that even a weak toroidal magnetic field can lead to MRI development which leads to the suppression of the large-scale modes. Notice also that the magneto-rotational instability in the disks is important because disks can be locally HD stable (according to Rayleigh criterion), but they are unstable for MHD local instability which is linear and independent by the field strength and orientation, and growing up on dynamical time scales. The torus (flow) is MHD turbulent due to the MRI.
We note that, with particular symmetries of the background (static) if we set \(B^r=0\) from the Maxwell equations, we infer \( B^{\theta }\cot \theta =0 \) (with \(\ell =\)constant), that is satisfied for \(B^{\theta }=0\) or \(\theta =\pi /2\).
The ratio \({\mathscr {M}}/\omega \) gives the comparison between the magnetic contribution to the fluid dynamics, through \( {\mathscr {M}}\), and the hydrodynamic contribution through its specific enthalpy \(\omega \).
For the hydrodynamic case the squeezing function \(R_s\) for the Schwarzschild background increases monotonically with K, and at fixed K decreases with \(\ell ^2\). This therefore means that the toroidal surface is squeezed on the equatorial plane with decreasing “energy” K and increasing \(\ell ^2\)—[20]. However this trend is reversed, that is \(R_s=h/\lambda <1\) reaching a minimum values of \(R_s\approx 0.95\), for increasing values of K, the squeezing decreases, or decreases until it reaches a minimum and then increases. In the magnetic case, the influence of the magnetic field has to be evaluated through the parameter \({\mathscr {S}}\). In general, as for the case \({\mathscr {S}}=0\), the torus is thicker as the K parameter increases, and becomes thinner as fluid angular momentum increases. Furthermore \(R_s\) increases with \({\mathscr {S}}\). For a small region of values of \(\ell \), the torus becomes thinner with increasing of \({\mathscr {S}}\) and viceversa becomes thicker with decreasing \({\mathscr {S}}\).
The Baumgarte-Shapiro-Shibata-Nakamura (BSSN) formalism, also known as BSSNOK [121] consists in a modification of the ADM formalism of General Relativity (in Hamiltonian formalism not making possible long term and stable numerical simulations)—[120]. The modification introduced in the ADM equations by the BSSN formalism includes consists essentially in the introduction of the auxiliary variables (to be considered with the extrinsic curvature and the three metric). Such change has been used for (long term) analysis of linear and non-linear gravitational waves or black holes pair collision and generally different physics of spinning and double BH systems or neutron stars and merging of neutron stars, collapse of spinning stars leading to a BH solutions.
Considering the BSSN formulation for the problem of weak hyperbolicity in the ADM equations, we also mention recent work [175] regarding the hyperbolicity of the \(3+1\) Valencia formulation of GRMHD when the solenoidal magnetic field constraint is enforced using hyperbolic divergence cleaning or presenting a vector potential formulations for GRMHD. Based on a dual-frame approach, the formulation for various fluid models is proved strongly hyperbolic, admitting consequently a well-posed initial value problem. The formulation with evolving vector potential is considered, and reducing to first-order it can be also strongly hyperbolic. The ideal GRMHD was consider in the Valencia flux-balance law form (but the equation were proved to be weakly hyperbolic therefore constituting an ill-posed initial value problem). Then GRMHD system in the hyperbolic divergence cleaning formulation and vector potential formulation results both strongly hyperbolic depending on sound speed (\(c_s\in ]0,1[\) or \(c_s\in ]0,1]\)).
We consider the method reviewed here a useful tool to establish uniqueness and stability properties although not applied in the formulation of numerical fully relativity code simulations. The first order formulations certainly represent a clear simplification in many contexts and are generally preferred in numerical computations as well as in the analysis of the motion of isolated bodies. Nevertheless, we mention that in [140] the local existence result for isolated dust (charged and uncharged) bodies based on a mixed order formulation has been provided. While, in [141, 142] the evolution equations for the EME system were first considered from the perspective from the Cauchy problem, where non-linear wave equations for the metric tensor describing the gravitational field adopting wave coordinates are obtained. However as consequence of this choice the evolution system is of mixed order (in [142] where Leray theory was implemented). More general discussions of the problem of the well-posedness of the evolution equations of the EME system and of MHD can be found in [143,144,145,146,147,148]. Then, the initial boundary value problem is a further relevant issue to be discussed, for example for the class of maximally dissipative boundary conditions used in [149], to show the well-posedness of the initial boundary problem for the vacuum Einstein field equations.
Note, we saw in Sects. 2 and 3 how, in the case of gravitating toroids, using some symmetries of the background and the matter and fields adapted to the geometry background and the accretion orbiting disks, the evolution equations were automatically satisfied leading to the development of a constrain model for the constraining equations for the matter capable to provide a good approximation for the analysis of a variety of orbiting accreting disks.
First simple method can be for example the Descartes criterion to determine the maximum number of positive and negative real roots of the characteristic polynomial and in particular simple cases one can make use of the so-called Routh–Hurwitz criterion to determine the number of roots with positive and negative real part of the polynomial by constructing the Routh associated matrix.
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Pugliese, D., Montani, G. Aspects of GRMHD in high-energy astrophysics: geometrically thick disks and tori agglomerates around spinning black holes. Gen Relativ Gravit 53, 51 (2021). https://doi.org/10.1007/s10714-021-02820-4
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DOI: https://doi.org/10.1007/s10714-021-02820-4