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(→‎Massless Polytropic Tori: Add comments to PP84 derivation in order to blend in later with Kojima's discussion)
(→‎Massless Polytropic Tori: Point to separate discussion of the Blaes (1985) paper.)
 
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=Massless Polytropic Tori=
=Massless Polytropic Tori=
(''aka'' Palapoizou-Pringle Tori)
(''aka'' Papaloizou-Pringle Tori)




[[Image:LSU_Structure_still.gif|74px|left]]
[[Image:LSU_Structure_still.gif|74px|left]]
In a seminal paper that focused on an analysis of nonaxisymmetric instabilities in accretion disks, [http://adsabs.harvard.edu/abs/1984MNRAS.208..721P Papaloizou & Pringle] (1984, MNRAS, 208, 721-750; hereafter, PP84) began by constructing equilibrium structures of axisymmetric, polytropic tori that reside in (orbit about) a point-mass potential.  The derived structures have analytic prescriptions.  Although the tori constructed by PP84 were not self-gravitating — ''i.e.'', the tori were ''massless'' — it is nevertheless instructive for us to examine how these equilibrium structures were derived.
In a seminal paper that focused on an analysis of nonaxisymmetric instabilities in accretion disks, [http://adsabs.harvard.edu/abs/1984MNRAS.208..721P Papaloizou & Pringle] (1984, MNRAS, 208, 721-750; hereafter, PP84) began by constructing equilibrium structures of axisymmetric, polytropic tori that reside in (orbit about) a Newtonian point-mass potential.  The derived structures have analytic prescriptions.  Although the tori constructed by PP84 were not self-gravitating — ''i.e.'', the tori were ''massless'' — it is nevertheless instructive for us to examine how these equilibrium structures were derived.
 
It is not widely appreciated that the equilibrium structure of Papaloizou-Pringle tori was first derived by [http://adsabs.harvard.edu/abs/1976ApJ...207..962F Fishbone & Moncrief (1976), ApJ, 207, 962] in a paper whose primary aim was to analyze the properties of thick disks orbiting around Kerr black holes.  In §IV of their paper, Fishbone & Moncrief show what thick-disk structures result ''in the Newtonian limit'' for homentropic systems with uniform specific angular momentum. These toroidal structures are identical to the ones whose stability was analyzed in PP84.  After reviewing the PP84 derivation, [[#Fishbone_.26_Moncrief_.281976.29|we present the Fishbone & Moncrief (1976) description]] of these equilibrium systems.


==Governing Relations==
==Governing Relations==
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As has been derived [[User:Tohline/AxisymmetricConfigurations/SolutionStrategies|elsewhere]], for axisymmetric configurations that obey a barotropic equation of state, hydrostatic balance is governed by the following ''algebraic'' expression:
As has been derived [[User:Tohline/AxisymmetricConfigurations/SolutionStrategies|elsewhere]], for axisymmetric configurations that obey a barotropic equation of state, hydrostatic balance is governed by the following ''algebraic'' expression:
<div align="center">
<div align="center">
<math>H + \Phi_\mathrm{eff} = C_\mathrm{B} ,</math>
<math>~H + \Phi_\mathrm{eff} = C_\mathrm{B} ,</math>
</div>
</div>
where <math>C_\mathrm{B}</math> is the Bernoulli constant,
where <math>~C_\mathrm{B}</math> is the Bernoulli constant,
<div align="center">
<div align="center">
<math>\Phi_\mathrm{eff} \equiv \Phi + \Psi ,</math>
<math>\Phi_\mathrm{eff} \equiv \Phi + \Psi ,</math>
</div>
</div>
and <math>\Psi</math> is the relevant centrifugal potential.  For self-gravitating configurations, this algebraic expression must be satisfied in concert with a self-consistent solution of the Poisson equation, but for the ''massless'' PP84 toroidal structures, {{User:Tohline/Math/VAR_NewtonianPotential01}} is just the Newtonian potential presented by a point-like object of mass <math>M_\mathrm{pt}</math>, namely,  
and <math>~\Psi</math> is the relevant centrifugal potential.  For self-gravitating configurations, this algebraic expression must be satisfied in concert with a self-consistent solution of the Poisson equation, but for the ''massless'' PP84 toroidal structures, {{User:Tohline/Math/VAR_NewtonianPotential01}} is just the Newtonian potential presented by a point-like object of mass <math>~M_\mathrm{pt}</math>, namely,  
<div align="center">
<div align="center">
<math>\Phi = - \frac{GM_\mathrm{pt}}{(\varpi^2 + z^2)^{1/2}} .</math>
<math>\Phi = - \frac{GM_\mathrm{pt}}{(\varpi^2 + z^2)^{1/2}} .</math>
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Inverting the first of these two expressions allows us to immediately derive the density distribution <math>\rho(\varpi,z)</math> throughout the torus from the derived algebraic expression for <math>H(\varpi,z)</math>.  Different density distributions will be obtained for different selected polytropic indexes and/or for different selected functional forms of the centrifugal potential.  
Inverting the first of these two expressions allows us to immediately derive the density distribution <math>\rho(\varpi,z)</math> throughout the torus from the derived algebraic expression for <math>H(\varpi,z)</math>.  Different density distributions will be obtained for different selected polytropic indexes and/or for different selected functional forms of the centrifugal potential.  


Here, also following PP84, we impose a steady-state velocity flow-field that is described by a fluid with uniform specific angular momentum, <math>j_0</math>.  Drawing from our table of example [[User:Tohline/AxisymmetricConfigurations/SolutionStrategies#SRPtable|''simple rotation profiles'']], the centrifugal potential that describes this chosen flow-field is given by the expression,
Here, also following PP84, we impose a steady-state velocity flow-field that is described by a fluid with uniform specific angular momentum, <math>~j_0</math>.  Drawing from our table of example [[User:Tohline/AxisymmetricConfigurations/SolutionStrategies#SRPtable|''simple rotation profiles'']], the centrifugal potential that describes this chosen flow-field is given by the expression,
<div align="center"><font size="+1">
<div align="center"><font size="+1">
<math>  
<math>  
Line 60: Line 62:
</div>  
</div>  
This is identical to Eq. (2.8) of PP84.
This is identical to Eq. (2.8) of PP84.




==Solution==
==Solution==


As PP84 point out, for these toroidal structures it is convenient to normalize all lengths to the position in the equatorial plane, <math>\varpi_0</math>, at which a fluid particle with specific angular momentum <math>j_0</math> has an angular orbital frequency, <math>\dot\varphi = j_0/\varpi^2</math>, that matches the Keplerian orbital frequency associated with the point-mass, <math>M_\mathrm{pt}</math>,  
As PP84 point out, for these toroidal structures it is convenient to normalize all lengths to the position in the equatorial plane, <math>~\varpi_0</math>, at which a fluid particle with specific angular momentum <math>~j_0</math> has an angular orbital frequency, <math>~\dot\varphi = j_0/\varpi^2</math>, that matches the Keplerian orbital frequency associated with the point-mass, <math>~M_\mathrm{pt}</math>,  
<div align="center">
<div align="center">
<math>
<math>
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</div>
</div>


It is worth noting that, in terms of the dimensionless radial coordinate <math>\chi</math>, the angular velocity and azimuthal velocity at any point inside the torus are, respectively,
It is worth noting that, in terms of the dimensionless radial coordinate <math>~\chi</math>, the angular velocity and azimuthal velocity at any point inside the torus are, respectively,
<div align="center">
<div align="center">
<math>
<math>
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</math>
</math>
</div>
</div>
where <math>\omega_K|_0 = (GM_\mathrm{pt} \varpi_0^{-3})^{1/2}</math> is the Keplerian frequency at <math>\varpi_0</math>and <math>v_\varphi|_0 = (GM_\mathrm{pt} \varpi_0^{-1})^{1/2}</math> is the azimuthal velocity at <math>\varpi_0</math>.
where <math>\omega_K|_0 = (GM_\mathrm{pt} \varpi_0^{-3})^{1/2}</math> is the Keplerian frequency at <math>\varpi_0</math> and <math>v_\varphi|_0 = (GM_\mathrm{pt} \varpi_0^{-1})^{1/2}</math> is the azimuthal velocity at <math>\varpi_0</math>.


===Pressure Maximum===
===Pressure Maximum===
It is instructive to examine at what location inside the torus the enthalpy (and density and gas pressure) assumes its maximum value.  At any radial location, <math>\chi_i</math>, <math>H</math> has a vertical maximum where  <math>\partial H/\partial\zeta = 0.</math>  That is, the maximum occurs where,
It is instructive to examine at what location inside the torus the enthalpy (and density and gas pressure) assumes its maximum value.  At any radial location, <math>~\chi_i</math>, <math>~H</math> has a vertical maximum where  <math>~\partial H/\partial\zeta = 0.</math>  That is, the maximum occurs where,
<div align="center">
<div align="center">
<math>
<math>
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</math>
</math>
</div>  
</div>  
For all values of <math>\chi_i</math>, this relation will be satisfied only at <math>\zeta = 0</math>.  Hence, vertically, the enthalpy maximum will be located in the equatorial plane of the torus.  Examining the radial enthalpy profile in the equatorial plane, we realize that the enthalpy maximum will occur where,
For all values of <math>~\chi_i</math>, this relation will be satisfied only at <math>~\zeta = 0</math>.  Hence, vertically, the enthalpy maximum will be located in the equatorial plane of the torus.  Examining the radial enthalpy profile in the equatorial plane, we realize that the enthalpy maximum will occur where,
<div align="center">
<div align="center">
<math>
<math>
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</math>
</math>
</div>  
</div>  
This relation will be satisfied only at <math>\chi = \varpi/\varpi_0 = 1</math>.  Hence, <math>\varpi_0</math> is not only the radial location (in the equatorial plane) where the angular frequency of the torus equals the Keplerian frequency, it is also the radial location of the pressure maximum.   
This relation will be satisfied only at <math>~\chi = \varpi/\varpi_0 = 1</math>.  Hence, <math>~\varpi_0</math> is not only the radial location (in the equatorial plane) where the angular frequency of the torus equals the Keplerian frequency, it is also the radial location of the pressure maximum.   


Note that the enthalpy at the pressure maximum &#8212; that is, at the location <math>~(\chi,\zeta) = (1,0)</math> &#8212; is,
<div align="center">
<math>
H_0 = (n+1)\biggl[ \frac{P}{\rho} \biggr]_0 = \frac{GM_\mathrm{pt}}{\varpi_0} \biggl[ \frac{1}{2}  - C_\mathrm{B}^' \biggr]  = \frac{(v_\varphi |_0)^2}{2} [1 - 2C_\mathrm{B}^' ] \, .
</math>
</div>


===Boundary Conditions===
===Boundary Conditions===


[[File:LSU_PP84Tori.jpg|right|400px|Meridional contours of constant <math>C_\mathrm{B}^'</math>.]] 
In the equatorial plane, the locations of the inner and outer edges of the torus are obtained by setting both <math>~H</math> and <math>~\zeta</math> to zero, that is, they are obtained from the roots of the equation,
In the equatorial plane, the locations of the inner and outer edges of the torus are obtained by setting both <math>H</math> and <math>\zeta</math> to zero, that is, they are obtained from the roots of the equation,
<div align="center">
<div align="center">
<math>
<math>
\chi^{-2} - 2\chi^{-1} + 2C_\mathrm{B}^' = 0  ,
~\chi^{-2} - 2\chi^{-1} + 2C_\mathrm{B}^' = 0  ,
</math>
</math>
</div>
</div>
that is, the inner <math>(\chi_-)</math> and outer <math>(\chi_+)</math> edges are located at,
that is, the inner <math>~(\chi_-)</math> and outer <math>~(\chi_+)</math> edges are located at,
<div align="center">
<div align="center">
<math>
<math>
\chi_\pm  =  \frac{1}{1 \mp \sqrt{1-2C_\mathrm{B}^'}} .
~\chi_\pm  =  \frac{1}{1 \mp \sqrt{1-2C_\mathrm{B}^'}} .
</math>
</math>
</div>
</div>
Clearly, the relative cross-sectional size &#8212; or, as defined in PP84, the dimensionless distortion parameter <math>\delta \equiv (\chi_+ + \chi_-)/2 = (2C_\mathrm{B}^')^{-1}</math> &#8212; is determined by the choice of the dimensionless Bernoulli constant, which must lie in the range, &frac12; <math> \geq C_\mathrm{B}^' \geq 0</math>.  For later reference, we will also note that the ratio of the inner edge to the outer edge is,
Clearly, the relative cross-sectional size &#8212; or, as defined in PP84, the dimensionless distortion parameter <math>~\delta \equiv (\chi_+ + \chi_-)/2 = (2C_\mathrm{B}^')^{-1}</math> &#8212; is determined by the choice of the dimensionless Bernoulli constant, which must lie in the range, <math>~\tfrac{1}{2} \geq C_\mathrm{B}^' \geq 0</math>.  For later reference, we will also note that the ratio of the inner edge to the outer edge is,
<div align="center">
<div align="center">
<math>
<math>
\frac{\chi_{-}}{\chi_{+}}  =  \frac{ 1 - \sqrt{1-2C_\mathrm{B}^'} }{1 + \sqrt{1-2C_\mathrm{B}^'} } .
~\frac{\chi_{-}}{\chi_{+}}  =  \frac{ 1 - \sqrt{1-2C_\mathrm{B}^'} }{1 + \sqrt{1-2C_\mathrm{B}^'} } .
</math>
</math>
</div>
</div>


Indeed, more generally, at all vertical locations above and below the equatorial plane, the surface of the torus occurs where the enthalpy goes to zero.  The meridional <math>(\chi,\zeta)</math> cross-section through three such surfaces are displayed in the accompanying figure.  The displayed surfaces correspond to <math>C_\mathrm{B}^' =</math> 0.208 (red curve), 0.276 (blue curve), and 0.373 (gold curve).  Carrying forward the above discussion, we note that in all three cases the pressure maximum is located at <math>(\chi,~\zeta) = (1,~0)</math>.  Properties of these tori are described in more detail in an accompanying discussion entitled, [[User:Tohline/Appendix/Ramblings/ToroidalCoordinates#Papaloizou-Pringle_Tori|''Toroidal Configurations and Related Coordinate Systems'']].   
Indeed, more generally, at all vertical locations above and below the equatorial plane, the surface of the torus occurs where the enthalpy goes to zero.  The meridional <math>~(\chi,\zeta)</math> cross-section through three such surfaces are displayed in the left panel of Figure 1.  The displayed surfaces correspond to <math>~C_\mathrm{B}^' =</math> 0.208 (red curve), 0.276 (blue curve), and 0.373 (green curve).  Carrying forward the above discussion, we note that in all three cases the pressure maximum is located at <math>(\chi,~\zeta) = (1,~0)</math>.  Properties of these tori are described in more detail in an accompanying discussion entitled, [[User:Tohline/Appendix/Ramblings/ToroidalCoordinates#Papaloizou-Pringle_Tori|''Toroidal Configurations and Related Coordinate Systems'']].   


We should perhaps emphasize that the shape of the surface of each torus, as shown in the accompanying figure, is independent of the chosen polytropic index.
We should perhaps emphasize that the shape of the surface of each torus, as shown in the left-hand panel of Figure 1, is independent of the chosen polytropic index.
 
 
<div align="center">
<table border="1" cellpadding="8" align="center" width="80%">
<tr><th align="center" colspan="2">Figure 1:  Papaloizou-Pringle Torus</th></tr>
<tr><td align="center">
[[File:LSU_PP84Tori.jpg|350px|Meridional contours of constant <math>C_\mathrm{B}^'</math>.]] 
</td>
<td align="center" bgcolor="#D0FFFF">
[[File:TorusMovie1.gif|350px|Pivoting PP Torus]]
</td></tr>
<tr>
  <td align="left">''Left Panel'' &#8212; A meridional cross-section outlining the surface of three separate PP tori:  <math>~C_\mathrm{B}^' =</math> 0.208 (red curve), 0.276 (blue curve), and 0.373 (green curve).</td>
  <td align="left">''Right Panel'' &#8212; A three-dimensional, cutaway rendering illustrating the geometric structure of one PP torus having <math>~C_\mathrm{B}^' = 0.3239,~</math><math>~x_\mathrm{in} = \chi_{-}/\chi_{+} = 0.2551, ~</math>&nbsp;<math>~x_0 = 0.4065.</math> The separately colored contours illustrate four surfaces of constant enthalpy; the red contour identifies the toroidal surface.</td>
</tr>
</table>
</div>


===Model as Described by Kojima===
===Model as Described by Kojima===
From the above expression for <math>\chi_\pm</math>, we see that,
From the above expression for <math>~\chi_\pm</math>, we see that,
<div align="center">
<div align="center">
<math>
<math>
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</math>
</math>
</div>
</div>
This agrees with the relation between <math>\chi_+</math> (written as <math>r_+</math>) and <math>\chi_-</math> (written as <math>r_-</math>) presented as equation (7) by [http://http://ptp.ipap.jp/link?PTP/75/251/ Kojima] (1986, Progress of Theoretical Physics, 75, 251-261), who also has examined the properties of Papaloizou-Pringle tori.  In his equation (8), Kojima points out that the inner edge of the torus lies within the range, &frac12; <math>< \chi_- < 1</math>, which is consistent with stating that the value of PB84's Bernoulli constant falls within the range, &frac12; <math> \geq C_\mathrm{B}^' \geq 0</math>.  Kojima also points out that, at the pressure maximum (see his equation 11),
This agrees with the relation between <math>~\chi_+</math> (written as <math>~r_+</math>) and <math>~\chi_-</math> (written as <math>~r_-</math>) presented as equation (7) by [http://http://ptp.ipap.jp/link?PTP/75/251/ Kojima] (1986, Progress of Theoretical Physics, 75, 251-261), who also has examined the properties of Papaloizou-Pringle tori.  In his equation (8), Kojima points out that the inner edge of the torus lies within the range, <math>~\tfrac{1}{2} < \chi_- < 1</math>, which is consistent with stating that the value of PB84's Bernoulli constant falls within the range, <math> ~\tfrac{1}{2} \geq C_\mathrm{B}^' \geq 0</math>.   
 
Using the just-derived relationship between <math>~C_\mathrm{B}^'</math> and <math>~\chi_-</math>, we deduce that the enthalpy at the pressure maximum depends only on the choice of <math>~\chi_-</math> as follows:
<div align="center">
<div align="center">
<math>
<math>
\frac{c_s}{v_\phi} = \frac{1}{\sqrt{6}} \biggl(\frac{1}{\chi_-} - 1 \biggr) \, .
H_0 = (n+1)\biggl[ \frac{P}{\rho} \biggr]_0 = \frac{(v_\varphi |_0)^2}{2} \biggl[ \frac{1}{\chi_-} - 1 \biggr]^2 \, .
</math>
</div>
Under adiabatic conditions, the sound speed of a gas is given by the algebraic relation,
<div align="center">
<math>
c_s^2 = \gamma \biggl[\frac{P}{\rho}\biggr] \, ,
</math>
</math>
</div>
</div>
where <math>~\gamma</math> is the specified adiabatic exponent.  Hence, the expression just derived for <math>~H_0</math> also gives us the sound speed at the pressure maximum of the torus, namely,
<div align="center">
<math>
(c_s |_0)^2 = \frac{\gamma}{(n + 1)}  \frac{(v_\varphi |_0)^2}{2} \biggl[ \frac{1}{\chi_-} - 1 \biggr]^2 \, ,
</math>
</div>
that is,
<div align="center">
<math>
\frac{c_s|_0}{v_\varphi |_0} = \biggl[ \frac{\gamma}{2(n + 1)} \biggr]^{1/2} \biggl[ \frac{1}{\chi_-} - 1 \biggr] \, .
</math>
</div>
This matches Kojima's equation (11) with <math>~\chi_-</math> written in place of <math>~r_-</math>, namely,
<div align="center">
<math>
\biggl( \frac{c_s}{v_\varphi} \biggr)_0 = \frac{1}{\sqrt{6}} \biggl(\frac{1}{\chi_-} - 1 \biggr) \, ,
</math>
</div>
when one adopts Kojima's choice of <math>~\gamma = 4/3</math> and <math>~n = (\gamma - 1)^{-1} = 3</math>.


===Hachisu Self-Consistent Field Technique===
===Hachisu Self-Consistent Field Technique===
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</math>
</math>
</div>
</div>
This expression for the dimensionless enthalpy has two unknowns:  <math>j_\mathrm{HSCF}</math> and <math>C_\mathrm{HSCF}</math>.  Hence, two boundary points must be specified before a solution for <math>H_\mathrm{HSCF}(\varpi,z)</math> can be obtained.  In the HSCF technique, it is customary to specify the location of two points on the surface of the configuration, where by design <math>H=0</math>.  For toroidal configurations, it is furthermore customary for that specification to be where the inner and outer edges of the torus touch the equatorial plane.  By design, the outer edge is at <math>(x_\mathrm{HSCF}, ~z_\mathrm{HSCF}) = (1, ~0)</math>; the inner edge will be at <math>(x_\mathrm{HSCF}, ~z_\mathrm{HSCF}) = (x_{in}, ~0)</math>.  Setting <math>H_\mathrm{HSCF}=0</math> at both of these locations gives the following two algebraic relations,
This expression for the dimensionless enthalpy has two unknowns:  <math>~j_\mathrm{HSCF}</math> and <math>~C_\mathrm{HSCF}</math>.  Hence, two boundary points must be specified before a solution for <math>~H_\mathrm{HSCF}(\varpi,z)</math> can be obtained.  In the HSCF technique, it is customary to specify the location of two points on the surface of the configuration, where by design <math>~H=0</math>.  For toroidal configurations, it is furthermore customary for that specification to be where the inner and outer edges of the torus touch the equatorial plane.  By design, the outer edge is at <math>~(x_\mathrm{HSCF}, ~z_\mathrm{HSCF}) = (1, ~0)</math>; the inner edge will be at <math>(x_\mathrm{HSCF}, ~z_\mathrm{HSCF}) = (x_{in}, ~0)</math>.  Setting <math>~H_\mathrm{HSCF}=0</math> at both of these locations gives the following two algebraic relations,
<div align="center">
<div align="center">
<math>
<math>
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</div>
</div>


At what radial position in the equatorial plane,  <math>x_0</math>, is the pressure maximum located?  The pressure maximum is also the enthalpy maximum, so the answer is given by looking in the equatorial plane <math>(z_\mathrm{HSCF} = 0)</math> for the location where <math>dH_\mathrm{HSCF}/dx_\mathrm{HSCF} = 0</math>.  Since,
At what radial position in the equatorial plane,  <math>~x_0</math>, is the pressure maximum located?  The pressure maximum is also the enthalpy maximum, so the answer is given by looking in the equatorial plane <math>~(z_\mathrm{HSCF} = 0)</math> for the location where <math>~dH_\mathrm{HSCF}/dx_\mathrm{HSCF} = 0</math>.  Since,
<div align="center">
<div align="center">
<math>
<math>
Line 243: Line 293:
</math>
</math>
</div>
</div>
Hence, in terms of <math>x_{in}</math>,
Hence, in terms of <math>~x_{in}</math>,
<div align="center">
<div align="center">
<math>
<math>
Line 251: Line 301:


===Comparison===
===Comparison===
The solution derived by PP84 (presented above) is normalized such that the pressure maximum is always in the equatorial plane at radial coordinate <math>\chi = 1</math>, and tori of different thicknesses are constructed by specifying different values of the dimensionless Bernoulli constant, <math>C_\mathrm{B}^'</math>.  Using the HSCF approach, the position of the outer edge of the torus is fixed and tori of different thicknesses are selected by moving the inner edge, <math>x_{in}</math>, around.  In order to examine whether or not the two solutions are, in fact, the same, we will re-write the expression given above for <math>\chi_{-}/\chi_{+}</math> in terms of <math>x_{in}</math>.  In order to do this, we need to convert <math>C_\mathrm{HSCF}</math> to <math>C_\mathrm{B}^'</math>.  Based on their definitions, the ratio
The solution derived by PP84 (presented above) is normalized such that the pressure maximum is always in the equatorial plane at radial coordinate <math>~\chi = 1</math>, and tori of different thicknesses are constructed by specifying different values of the dimensionless Bernoulli constant, <math>~C_\mathrm{B}^'</math>.  Using the HSCF approach, the position of the outer edge of the torus is fixed and tori of different thicknesses are selected by moving the inner edge, <math>~x_{in}</math>, around.  In order to examine whether or not the two solutions are, in fact, the same, we will re-write the expression given above for <math>~\chi_{-}/\chi_{+}</math> in terms of <math>~x_{in}</math>.  In order to do this, we need to convert <math>~C_\mathrm{HSCF}</math> to <math>~C_\mathrm{B}^'</math>.  Based on their definitions, the ratio
<div align="center">
<div align="center">
<math>
<math>
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</div>
</div>
Hence, both the PP84 derivation and the HSCF derivation produce the same result.
Hence, both the PP84 derivation and the HSCF derivation produce the same result.
==Blaes (1985)==
In a [[User:Tohline/Appendix/Ramblings/PPTori#Blaes85|separate chapter]], we review the analytic analysis of unstable nonaxisymmetric eigenmodes in geometrically thin PP tori that has been presented by [http://adsabs.harvard.edu/abs/1985MNRAS.216..553B Blaes (1985), MNRAS, 216, 553].  Our review includes an explanation of how the [[#Solution|equations derived here]] to describe the equilibrium structure of PP Tori are straightforwardly transformed into the equations and notation adopted by Blaes.
{{LSU_WorkInProgress}}
==Fishbone &amp; Moncrief (1976)==
[http://adsabs.harvard.edu/abs/1976ApJ...207..962F Fishbone &amp; Moncrief (1976), ApJ, 207, 962] derived the identical Papaloizou-Pringle torus structure using a spherical rather than cylindrical coordinate system.
===Derived Equilibrium Structure ===
<div align="center">
<table border="0" cellpadding="5" align="center">
<tr>
  <td align="right">
<math>~c^2 \frac{\partial w}{\partial r} \equiv \frac{1}{(nm)} \frac{\partial P}{\partial r}</math>
  </td>
  <td align="center">
<math>~=</math>
  </td>
  <td align="left">
<math>~\frac{\partial}{\partial r}\biggl(\frac{GM}{r}\biggr) + \omega^2  r^2 \sin^2\theta \, ,</math>
  </td>
</tr>
<tr>
  <td align="right">
<math>~c^2 \frac{\partial w}{\partial \theta} \equiv \frac{1}{(nm)} \frac{\partial P}{\partial \theta}</math>
  </td>
  <td align="center">
<math>~=</math>
  </td>
  <td align="left">
<math>~\frac{\partial}{\partial \theta}\biggl(\frac{GM}{r}\biggr) + \omega^2  r^2 \sin\theta \cos\theta \, .</math>
  </td>
</tr>
</table>
</div>
As presented in their equation (4.4), imposing the condition of uniform specific angular momentum leads to an angular velocity profile of the form,
<div align="center">
<math>~\omega = \frac{\ell}{r^2 \sin^2\theta} \, .</math>
</div>
===Comparison===
=Key References=
* [http://adsabs.harvard.edu/abs/1976ApJ...207..962F Fishbone &amp; Moncrief (1976), ApJ, 207, 962] &#8212; ''Relativistic fluid disks in orbit around Kerr black holes''
* [http://adsabs.harvard.edu/abs/1984MNRAS.208..721P Papaloizou &amp; Pringle (1984), MNRAS, 208, 721] &#8212; ''The dynamical stability of differentially rotating discs with constant specific angular momentum''
* [http://adsabs.harvard.edu/abs/1985MNRAS.213..799P Papaloizou &amp; Pringle (1985), MNRAS, 213, 799] &#8212; ''The dynamical stability of differentially rotating discs. &nbsp; II.''
* [http://adsabs.harvard.edu/abs/1987MNRAS.225..267P Papaloizou &amp; Pringle (1987), MNRAS, 225, 267] &#8212; ''The dynamical stability of differentially rotating discs. &nbsp; III.''
* [http://adsabs.harvard.edu/abs/1985MNRAS.213P...7G Goldreich &amp; Narayan (1985), MNRAS, 213, 7] &#8212; ''Non-axisymmetric instability in thin discs''
* [http://adsabs.harvard.edu/abs/1986MNRAS.221..339G Goldrich, Goodman &amp; Narayan (1986), MNRAS, 221, 339] &#8212; ''The stability of accretion tori. &nbsp; I. -- Long-wavelength modes of slender tori''
* [http://adsabs.harvard.edu/abs/1987MNRAS.225..695G Goodman, Narayan, &amp; Goldreich (1987), MNRAS, 225, 695] &#8212; ''The stability of accretion tori. &nbsp; II -- Non-linear evolution to discrete planets''
* [http://adsabs.harvard.edu/abs/1988MNRAS.231...97G Goodman &amp; Narayan (1988), MNRAS, 231, 97] &#8212; ''The stability of accretion tori. &nbsp; III -- The effect of self-gravity''
* [http://adsabs.harvard.edu/abs/1992ApJ...388..451C Christodoulou &amp; Narayan (1992), ApJ, 388, 451] &#8212; ''The stability of accretion tori. &nbsp; IV. Fission and fragmentation of slender, self-gravitating annuli''
* [http://adsabs.harvard.edu/abs/1993ApJ...412..696C Christodoulou (1993), ApJ, 412, 696] &#8212; ''The stability of accretion tori. &nbsp; V. Unstable modes and avoided crossings in extended, self-gravitating annuli''
* [http://adsabs.harvard.edu/abs/1986MNRAS.221..279R Robertson &amp; Frank (1986), MNRAS, 221, 279] &#8212; ''A numerical study of two-dimensional accretion flows''
* [http://adsabs.harvard.edu/abs/1988MNRAS.232....1F Frank &amp; Robertson (1988), MNRAS, 232, 1] &#8212; ''Numerical studies of the dynamical stability of differentially rotating tori''
* [http://adsabs.harvard.edu/abs/1985MNRAS.216..553B Blaes (1985), MNRAS, 216, 553] &#8212; ''Oscillations of slender tori''
* [http://adsabs.harvard.edu/abs/1986PThPh..75..251K Kojima (1986), PThPh, 75, 251] &#8212; ''The Dynamical Stability of a Fat Disk with Constant Specific Angular Momentum''
* [http://adsabs.harvard.edu/abs/1989MNRAS.236..589K Kojima (1989), MNRAS, 236, 589] &#8212; ''Non-axisymmetric unstable modes of a differentially rotating torus''
* [http://adsabs.harvard.edu/abs/1986MNRAS.223..859H Hanawa (1986), MNRAS, 223, 859] &#8212; ''Dynamical instability of a homoentropic rotating torus and an upper limit on the growth rate''
* [http://adsabs.harvard.edu/abs/1987MNRAS.225..677H Hawley (1987), MNRAS, 225, 677] &#8212; ''Non-linear evolution of a non-axisymmetric disc instability''
* [http://adsabs.harvard.edu/abs/1988ApJ...326..277B Blaes &amp; Hawley (1988), ApJ, 326, 277] &#8212; ''Nonaxisymmetric disk instabilities -- A linear and nonlinear synthesis''
* [http://adsabs.harvard.edu/abs/1990ApJ...356..580H Hawley (1990), ApJ, 356, 580] &#8212; ''Nonaxisymmetric instabilities in a slender torus -- Two- and three-dimensional simulations''
* [http://adsabs.harvard.edu/abs/1988MNRAS.231..739B Boss (1988), MNRAS, 231, 739] &#8212; ''Non-axisymmetric instability in three-dimensional accretion toroids''
* [http://adsabs.harvard.edu/abs/1989ApJ...344..645P Papaloizou &amp; Lin (1989), ApJ, 344, 645] &#8212; ''Nonaxisymmetric instabilities in thin self-gravitating rings and disks''
* [http://adsabs.harvard.edu/abs/1991MNRAS.248..353P Papaloizou &amp; Savonije (1991), MNRAS, 248, 353] &#8212; ''Instabilities in self-gravitating gaseous discs''
* [http://adsabs.harvard.edu/abs/1995ARA%26A..33..505P Papaloizou &amp; Lin (1995), <font color="red">Annual Reviews of Astronomy &amp; Astrophysics</font>, 33, 505] &#8212; ''Theory of Accretion Disks I:  Angular Momentum Transport Processes''
* [http://adsabs.harvard.edu/abs/1990ApJ...361..394T Tohline &amp; Hachisu (1990), ApJ, 361, 394] &#8212; ''The breakup of self-gravitating rings, tori, and thick accretion disks''
* [http://adsabs.harvard.edu/abs/1994ApJ...420..247W Woodward, Tohline &amp; Hachisu (1994), ApJ, 420, 247] &#8212; ''The stability of thick, self-gravitating disks in protostellar systems''
* [http://adsabs.harvard.edu/abs/1997ApJS..108..471A Andalib, Tohline, &amp; Christodoulou (1997), ApJS, 108, 471] &#8212; ''A Survey of the Principal Modes of Nonaxisymmetric Instability in Self-Gravitating Accretion Disk Models''
* [http://adsabs.harvard.edu/abs/2011Ap%26SS.334....1H Hadley &amp; Imamura (2011), Ap&amp;SS, 334, 1] &#8212; ''Nonaxisymmetric instabilities of self-gravitating disks. &nbsp; I. Toroids''
* [http://adsabs.harvard.edu/abs/2014Ap%26SS.353..191H Hadley, Fernandez, Imamura, Keever, Tumblin, &amp; Dumas (2014), Ap&amp;SS, 353, 191]&#8212; ''Nonaxisymmetric instabilities in self-gravitating disks. &nbsp; II. Linear and quasi-linear analysis''
* [http://adsabs.harvard.edu/abs/2015Ap%26SS.359...10H Hadley, Dumas, Imamura, Keever &amp; Tumblin (2015), Ap&amp;SS, 359, 10]&#8212; ''Nonaxisymmetric instabilities in self-gravitating disks. &nbsp; III. Angular momentum transport''
----
* [http://adsabs.harvard.edu/abs/1985A%26A...149..487B Balbinski (1985), AA, 149, 487] &#8212; ''The character of the normal mode equationos for rotating perfect fluids''
* [http://adsabs.harvard.edu/abs/1990MNRAS.245..614L P. J. Luyten (1990), MNRAS, 245, 614] &#8212; ''Non-Axisymmetric Dynamical Instability of Differentially Rotating Self-Gravitating Masses''
* [http://adsabs.harvard.edu/abs/1993GApFD..70..235D Bubrulle, Chomaz, Kumar, &amp; Rieutord (1993), Geophysical and Astrophysical Fluid Dynamics, 70, 235] &#8212; ''Non linear stability of slender accretion disks by bifurcation method''
* [http://adsabs.harvard.edu/abs/1995ChA%26A..19..507L Liu &amp; Wang (1995), ChA&amp;A, 19, 507] &#8212; ''A numerical solution of the dynamical instability of a thin accretion torus''
* [http://adsabs.harvard.edu/abs/2002RSPSA.458..359B Beyer (2002), RSPSA, 458, 359] &#8212; ''A framework for perturbations and stability of differentially rotating stars''
* [http://adsabs.harvard.edu/abs/2004MNRAS.350..927W Watts, Andersson, &amp; Williams (2004), MNRAS, 350, 927] &#8212; ''The oscillation and stability of differentially rotating spherical shells:  the initial-value problem''
* [http://adsabs.harvard.edu/abs/2015MNRAS.446..555P Passamonti &amp; Andersson (2015), MNRAS, 446, 555] &#8212; ''The intimate relation between the low T/W instability and the corotation point''


=Related Wikipedia Discussions=
=Related Wikipedia Discussions=

Latest revision as of 20:45, 26 February 2016

Whitworth's (1981) Isothermal Free-Energy Surface
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Massless Polytropic Tori

(aka Papaloizou-Pringle Tori)


LSU Structure still.gif

In a seminal paper that focused on an analysis of nonaxisymmetric instabilities in accretion disks, Papaloizou & Pringle (1984, MNRAS, 208, 721-750; hereafter, PP84) began by constructing equilibrium structures of axisymmetric, polytropic tori that reside in (orbit about) a Newtonian point-mass potential. The derived structures have analytic prescriptions. Although the tori constructed by PP84 were not self-gravitating — i.e., the tori were massless — it is nevertheless instructive for us to examine how these equilibrium structures were derived.

It is not widely appreciated that the equilibrium structure of Papaloizou-Pringle tori was first derived by Fishbone & Moncrief (1976), ApJ, 207, 962 in a paper whose primary aim was to analyze the properties of thick disks orbiting around Kerr black holes. In §IV of their paper, Fishbone & Moncrief show what thick-disk structures result in the Newtonian limit for homentropic systems with uniform specific angular momentum. These toroidal structures are identical to the ones whose stability was analyzed in PP84. After reviewing the PP84 derivation, we present the Fishbone & Moncrief (1976) description of these equilibrium systems.

Governing Relations

As has been derived elsewhere, for axisymmetric configurations that obey a barotropic equation of state, hydrostatic balance is governed by the following algebraic expression:

<math>~H + \Phi_\mathrm{eff} = C_\mathrm{B} ,</math>

where <math>~C_\mathrm{B}</math> is the Bernoulli constant,

<math>\Phi_\mathrm{eff} \equiv \Phi + \Psi ,</math>

and <math>~\Psi</math> is the relevant centrifugal potential. For self-gravitating configurations, this algebraic expression must be satisfied in concert with a self-consistent solution of the Poisson equation, but for the massless PP84 toroidal structures, <math>~\Phi</math> is just the Newtonian potential presented by a point-like object of mass <math>~M_\mathrm{pt}</math>, namely,

<math>\Phi = - \frac{GM_\mathrm{pt}}{(\varpi^2 + z^2)^{1/2}} .</math>

Hence, the enthalpy distribution <math>H(\varpi,z)</math> throughout the torus can be described analytically for any one of a number of different simple rotation profiles by plugging the appropriate expression for the associated centrifugal potential, <math>\Psi(\varpi)</math>, into the governing relation,

<math> H = -\Phi_\mathrm{eff} + C_\mathrm{B} = \frac{GM_\mathrm{pt}}{(\varpi^2 + z^2)^{1/2}} - \Psi + C_\mathrm{B} . </math>

Supplemental Relations

Following PP84, we supplement the above-specified set of governing equations with a polytropic equation of state, as defined in our overview of supplemental relations for time-independent problems. Specifically, we will assume that <math>~\rho</math> is related to <math>~H</math> through the relation,

<math>~H = (n+1)K_\mathrm{n} \rho^{1/n}</math> ,

or we can set,

<math> H = (n+1) \frac{P}{\rho} . </math>

Inverting the first of these two expressions allows us to immediately derive the density distribution <math>\rho(\varpi,z)</math> throughout the torus from the derived algebraic expression for <math>H(\varpi,z)</math>. Different density distributions will be obtained for different selected polytropic indexes and/or for different selected functional forms of the centrifugal potential.

Here, also following PP84, we impose a steady-state velocity flow-field that is described by a fluid with uniform specific angular momentum, <math>~j_0</math>. Drawing from our table of example simple rotation profiles, the centrifugal potential that describes this chosen flow-field is given by the expression,

<math> \Psi(\varpi) = \frac{j_0^2}{2\varpi^2} . </math>

Summary

Inserting the two supplemental relations into the governing algebraic expression for <math>H(\varpi,z)</math>, we conclude that the polytropic tori studied by PP84 must have structures that satisfy the equation,

<math> (n+1)\frac{P}{\rho} = \frac{GM_\mathrm{pt}}{(\varpi^2 + z^2)^{1/2}} - \frac{j_0^2}{2\varpi^2} + C_\mathrm{B} . </math>

This is identical to Eq. (2.8) of PP84.


Solution

As PP84 point out, for these toroidal structures it is convenient to normalize all lengths to the position in the equatorial plane, <math>~\varpi_0</math>, at which a fluid particle with specific angular momentum <math>~j_0</math> has an angular orbital frequency, <math>~\dot\varphi = j_0/\varpi^2</math>, that matches the Keplerian orbital frequency associated with the point-mass, <math>~M_\mathrm{pt}</math>,

<math> \omega_K \equiv \biggl[ \frac{GM_\mathrm{pt}}{\varpi^3} \biggr]^{1/2} . </math>

That is, it is convenient to define the dimensionless coordinates,

<math> \chi \equiv \frac{\varpi}{\varpi_0} ~~~~~\mathrm{and}~~~~~ \zeta \equiv \frac{z}{\varpi_0} , </math>

where,

<math> \varpi_0 \equiv \frac{j_0^2}{GM_\mathrm{pt}} . </math>

The algebraic relation defining the equilibrium structure then becomes,

<math> H = (n+1)\frac{P}{\rho} = \frac{GM_\mathrm{pt}}{\varpi_0} \biggl[ (\chi^2 + \zeta^2)^{-1/2} - \frac{1}{2}\chi^{-2} - C_\mathrm{B}^' \biggr] , </math>

where the normalized Bernoulli constant,

<math> C_\mathrm{B}^' \equiv - \frac{C_\mathrm{B} \varpi_0}{GM_\mathrm{pt}} . </math>

It is worth noting that, in terms of the dimensionless radial coordinate <math>~\chi</math>, the angular velocity and azimuthal velocity at any point inside the torus are, respectively,

<math> \dot\varphi = \chi^{-2} \omega_K |_0 \, , </math>

and,

<math> v_\varphi \equiv \varpi\dot\varphi = \chi^{-1} v_\varphi |_0 \, , </math>

where <math>\omega_K|_0 = (GM_\mathrm{pt} \varpi_0^{-3})^{1/2}</math> is the Keplerian frequency at <math>\varpi_0</math> and <math>v_\varphi|_0 = (GM_\mathrm{pt} \varpi_0^{-1})^{1/2}</math> is the azimuthal velocity at <math>\varpi_0</math>.

Pressure Maximum

It is instructive to examine at what location inside the torus the enthalpy (and density and gas pressure) assumes its maximum value. At any radial location, <math>~\chi_i</math>, <math>~H</math> has a vertical maximum where <math>~\partial H/\partial\zeta = 0.</math> That is, the maximum occurs where,

<math> \frac{\partial}{\partial\zeta} \biggl[ (\chi_i^2 + \zeta^2)^{-1/2} - \frac{1}{2}\chi_i^{-2} - C_\mathrm{B}^' \biggr] = -\zeta (\chi_i^2 + \zeta^2)^{-3/2} = 0 . </math>

For all values of <math>~\chi_i</math>, this relation will be satisfied only at <math>~\zeta = 0</math>. Hence, vertically, the enthalpy maximum will be located in the equatorial plane of the torus. Examining the radial enthalpy profile in the equatorial plane, we realize that the enthalpy maximum will occur where,

<math> \frac{\partial}{\partial\chi} \biggl[ \chi^{-1} - \frac{1}{2}\chi^{-2} - C_\mathrm{B}^' \biggr] = -\chi^{-2} + \chi^{-3} = 0 . </math>

This relation will be satisfied only at <math>~\chi = \varpi/\varpi_0 = 1</math>. Hence, <math>~\varpi_0</math> is not only the radial location (in the equatorial plane) where the angular frequency of the torus equals the Keplerian frequency, it is also the radial location of the pressure maximum.

Note that the enthalpy at the pressure maximum — that is, at the location <math>~(\chi,\zeta) = (1,0)</math> — is,

<math> H_0 = (n+1)\biggl[ \frac{P}{\rho} \biggr]_0 = \frac{GM_\mathrm{pt}}{\varpi_0} \biggl[ \frac{1}{2} - C_\mathrm{B}^' \biggr] = \frac{(v_\varphi |_0)^2}{2} [1 - 2C_\mathrm{B}^' ] \, . </math>

Boundary Conditions

In the equatorial plane, the locations of the inner and outer edges of the torus are obtained by setting both <math>~H</math> and <math>~\zeta</math> to zero, that is, they are obtained from the roots of the equation,

<math> ~\chi^{-2} - 2\chi^{-1} + 2C_\mathrm{B}^' = 0 , </math>

that is, the inner <math>~(\chi_-)</math> and outer <math>~(\chi_+)</math> edges are located at,

<math> ~\chi_\pm = \frac{1}{1 \mp \sqrt{1-2C_\mathrm{B}^'}} . </math>

Clearly, the relative cross-sectional size — or, as defined in PP84, the dimensionless distortion parameter <math>~\delta \equiv (\chi_+ + \chi_-)/2 = (2C_\mathrm{B}^')^{-1}</math> — is determined by the choice of the dimensionless Bernoulli constant, which must lie in the range, <math>~\tfrac{1}{2} \geq C_\mathrm{B}^' \geq 0</math>. For later reference, we will also note that the ratio of the inner edge to the outer edge is,

<math> ~\frac{\chi_{-}}{\chi_{+}} = \frac{ 1 - \sqrt{1-2C_\mathrm{B}^'} }{1 + \sqrt{1-2C_\mathrm{B}^'} } . </math>

Indeed, more generally, at all vertical locations above and below the equatorial plane, the surface of the torus occurs where the enthalpy goes to zero. The meridional <math>~(\chi,\zeta)</math> cross-section through three such surfaces are displayed in the left panel of Figure 1. The displayed surfaces correspond to <math>~C_\mathrm{B}^' =</math> 0.208 (red curve), 0.276 (blue curve), and 0.373 (green curve). Carrying forward the above discussion, we note that in all three cases the pressure maximum is located at <math>(\chi,~\zeta) = (1,~0)</math>. Properties of these tori are described in more detail in an accompanying discussion entitled, Toroidal Configurations and Related Coordinate Systems.

We should perhaps emphasize that the shape of the surface of each torus, as shown in the left-hand panel of Figure 1, is independent of the chosen polytropic index.


Figure 1: Papaloizou-Pringle Torus

Meridional contours of constant <math>C_\mathrm{B}^'</math>.

Pivoting PP Torus

Left Panel — A meridional cross-section outlining the surface of three separate PP tori: <math>~C_\mathrm{B}^' =</math> 0.208 (red curve), 0.276 (blue curve), and 0.373 (green curve). Right Panel — A three-dimensional, cutaway rendering illustrating the geometric structure of one PP torus having <math>~C_\mathrm{B}^' = 0.3239,~</math><math>~x_\mathrm{in} = \chi_{-}/\chi_{+} = 0.2551, ~</math> <math>~x_0 = 0.4065.</math> The separately colored contours illustrate four surfaces of constant enthalpy; the red contour identifies the toroidal surface.

Model as Described by Kojima

From the above expression for <math>~\chi_\pm</math>, we see that,

<math> \sqrt{1-2C_\mathrm{B}^'} = \frac{1}{\chi_-} - 1 = 1 - \frac{1}{\chi_+} \, . </math>

Hence,

<math> \chi_+ = \biggl[ 2 - \frac{1}{\chi_-}\biggr]^{-1} = \frac{\chi_-}{2\chi_- - 1} \, . </math>

This agrees with the relation between <math>~\chi_+</math> (written as <math>~r_+</math>) and <math>~\chi_-</math> (written as <math>~r_-</math>) presented as equation (7) by Kojima (1986, Progress of Theoretical Physics, 75, 251-261), who also has examined the properties of Papaloizou-Pringle tori. In his equation (8), Kojima points out that the inner edge of the torus lies within the range, <math>~\tfrac{1}{2} < \chi_- < 1</math>, which is consistent with stating that the value of PB84's Bernoulli constant falls within the range, <math> ~\tfrac{1}{2} \geq C_\mathrm{B}^' \geq 0</math>.

Using the just-derived relationship between <math>~C_\mathrm{B}^'</math> and <math>~\chi_-</math>, we deduce that the enthalpy at the pressure maximum depends only on the choice of <math>~\chi_-</math> as follows:

<math> H_0 = (n+1)\biggl[ \frac{P}{\rho} \biggr]_0 = \frac{(v_\varphi |_0)^2}{2} \biggl[ \frac{1}{\chi_-} - 1 \biggr]^2 \, . </math>

Under adiabatic conditions, the sound speed of a gas is given by the algebraic relation,

<math> c_s^2 = \gamma \biggl[\frac{P}{\rho}\biggr] \, , </math>

where <math>~\gamma</math> is the specified adiabatic exponent. Hence, the expression just derived for <math>~H_0</math> also gives us the sound speed at the pressure maximum of the torus, namely,

<math> (c_s |_0)^2 = \frac{\gamma}{(n + 1)} \frac{(v_\varphi |_0)^2}{2} \biggl[ \frac{1}{\chi_-} - 1 \biggr]^2 \, , </math>

that is,

<math> \frac{c_s|_0}{v_\varphi |_0} = \biggl[ \frac{\gamma}{2(n + 1)} \biggr]^{1/2} \biggl[ \frac{1}{\chi_-} - 1 \biggr] \, . </math>

This matches Kojima's equation (11) with <math>~\chi_-</math> written in place of <math>~r_-</math>, namely,

<math> \biggl( \frac{c_s}{v_\varphi} \biggr)_0 = \frac{1}{\sqrt{6}} \biggl(\frac{1}{\chi_-} - 1 \biggr) \, , </math>

when one adopts Kojima's choice of <math>~\gamma = 4/3</math> and <math>~n = (\gamma - 1)^{-1} = 3</math>.

Hachisu Self-Consistent Field Technique

For the sake of contextual continuity, it is useful to relate the above result to the Hachisu self-consistent field (HSCF) technique, which we rely upon heavily to derive the equilibrium structure of self-gravitating systems. The HSCF technique begins by identifying the relevant algebraic expression for the enthalpy as derived above, namely,

<math> H = \frac{GM_\mathrm{pt}}{(\varpi^2 + z^2)^{1/2}} - \frac{j_0^2}{2\varpi^2} + C_\mathrm{B} . </math>

In the HSCF technique, it is customary to normalize all lengths to the distance <math>\varpi_{+}</math> from the origin to the point where the outer edge of the torus touches the equatorial plane. From this perspective, then, the relevant dimensionless coordinates are,

<math> x_\mathrm{HSCF} \equiv \frac{\varpi}{\varpi_{+}} ~~~~~\mathrm{and}~~~~~ z_\mathrm{HSCF} \equiv \frac{z}{\varpi_{+}} , </math>

and the equation for the dimensionless enthalpy becomes,

<math> H_\mathrm{HSCF} \equiv \frac{H}{(GM_\mathrm{pt}/\varpi_{+})} = (x_\mathrm{HSCF}^2 + z_\mathrm{HSCF}^2)^{-1/2} - \frac{1}{2} (j_\mathrm{HSCF}^2) x_\mathrm{HSCF}^{-2} - C_\mathrm{HSCF} , </math>

where the normalized Bernoulli constant,

<math> C_\mathrm{HSCF} \equiv - \frac{C_\mathrm{B} \varpi_{+}}{GM_\mathrm{pt}} , </math>

and the normalized specific angular momentum is,

<math> j_\mathrm{HSCF} \equiv \frac{j_0}{(GM_\mathrm{pt} \varpi_{+})^{1/2}} . </math>

This expression for the dimensionless enthalpy has two unknowns: <math>~j_\mathrm{HSCF}</math> and <math>~C_\mathrm{HSCF}</math>. Hence, two boundary points must be specified before a solution for <math>~H_\mathrm{HSCF}(\varpi,z)</math> can be obtained. In the HSCF technique, it is customary to specify the location of two points on the surface of the configuration, where by design <math>~H=0</math>. For toroidal configurations, it is furthermore customary for that specification to be where the inner and outer edges of the torus touch the equatorial plane. By design, the outer edge is at <math>~(x_\mathrm{HSCF}, ~z_\mathrm{HSCF}) = (1, ~0)</math>; the inner edge will be at <math>(x_\mathrm{HSCF}, ~z_\mathrm{HSCF}) = (x_{in}, ~0)</math>. Setting <math>~H_\mathrm{HSCF}=0</math> at both of these locations gives the following two algebraic relations,

<math> C_\mathrm{HSCF} = 1 - \frac{1}{2} (j_\mathrm{HSCF}^2) , </math>

and

<math> C_\mathrm{HSCF} = x_{in}^{-1} - \frac{1}{2} (j_\mathrm{HSCF}^2) x_{in}^{-2} , </math>

which can be used in combination to solve for the two unknowns. The result is,

<math> C_\mathrm{HSCF} = \frac{1}{1 + x_{in}} , </math>

and,

<math> j_\mathrm{HSCF} = \biggl[ \frac{2x_{in}}{1 + x_{in}} \biggr]^{1/2} . </math>

At what radial position in the equatorial plane, <math>~x_0</math>, is the pressure maximum located? The pressure maximum is also the enthalpy maximum, so the answer is given by looking in the equatorial plane <math>~(z_\mathrm{HSCF} = 0)</math> for the location where <math>~dH_\mathrm{HSCF}/dx_\mathrm{HSCF} = 0</math>. Since,

<math> \frac{dH_\mathrm{HSCF}}{dx_\mathrm{HSCF}} = - x_\mathrm{HSCF}^{-2} + (j_\mathrm{HSCF}^2) x_\mathrm{HSCF}^{-3} \, , </math>

the pressure maximum must be located at,

<math> x_\mathrm{HSCF} = x_0 = j_\mathrm{HSCF}^2 \, . </math>

Hence, in terms of <math>~x_{in}</math>,

<math> x_0 = \frac{2x_{in}}{1 + x_{in}} . </math>

Comparison

The solution derived by PP84 (presented above) is normalized such that the pressure maximum is always in the equatorial plane at radial coordinate <math>~\chi = 1</math>, and tori of different thicknesses are constructed by specifying different values of the dimensionless Bernoulli constant, <math>~C_\mathrm{B}^'</math>. Using the HSCF approach, the position of the outer edge of the torus is fixed and tori of different thicknesses are selected by moving the inner edge, <math>~x_{in}</math>, around. In order to examine whether or not the two solutions are, in fact, the same, we will re-write the expression given above for <math>~\chi_{-}/\chi_{+}</math> in terms of <math>~x_{in}</math>. In order to do this, we need to convert <math>~C_\mathrm{HSCF}</math> to <math>~C_\mathrm{B}^'</math>. Based on their definitions, the ratio

<math> \frac{C_\mathrm{B}^'}{C_\mathrm{HSCF} } = \frac{\varpi_0}{\varpi_{+}} = x_0 . </math>

Hence,

<math> C_\mathrm{B}^' = x_0~C_\mathrm{HSCF} = \biggl( \frac{2x_{in}}{1+x_{in}} \biggr) \biggl( \frac{1}{1+x_{in}} \biggr) = \frac{2x_{in}}{(1+x_{in})^2}. </math>

Therefore,

<math> 1 - 2C_\mathrm{B}^' = 1 - \frac{4x_{in}}{(1+x_{in})^2} = \frac{ (1+x_{in})^2 - 4x_{in} }{(1+x_{in})^2} = \frac{ (1-x_{in})^2 }{(1+x_{in})^2} \, , </math>

and,

<math> \frac{\chi_{-}}{\chi_{+}} = \frac{ 1 - \sqrt{1-2C_\mathrm{B}^'} }{1 + \sqrt{1-2C_\mathrm{B}^'} } = \frac{ 1 - \frac{1-x_{in}}{1+x_{in}} }{1 + \frac{1-x_{in}}{1+x_{in}}} = \frac{ (1+x_{in}) - (1-x_{in}) }{ (1+x_{in}) + (1-x_{in}) } = x_{in}. </math>

Hence, both the PP84 derivation and the HSCF derivation produce the same result.

Blaes (1985)

In a separate chapter, we review the analytic analysis of unstable nonaxisymmetric eigenmodes in geometrically thin PP tori that has been presented by Blaes (1985), MNRAS, 216, 553. Our review includes an explanation of how the equations derived here to describe the equilibrium structure of PP Tori are straightforwardly transformed into the equations and notation adopted by Blaes.



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Fishbone & Moncrief (1976)

Fishbone & Moncrief (1976), ApJ, 207, 962 derived the identical Papaloizou-Pringle torus structure using a spherical rather than cylindrical coordinate system.

Derived Equilibrium Structure

<math>~c^2 \frac{\partial w}{\partial r} \equiv \frac{1}{(nm)} \frac{\partial P}{\partial r}</math>

<math>~=</math>

<math>~\frac{\partial}{\partial r}\biggl(\frac{GM}{r}\biggr) + \omega^2 r^2 \sin^2\theta \, ,</math>

<math>~c^2 \frac{\partial w}{\partial \theta} \equiv \frac{1}{(nm)} \frac{\partial P}{\partial \theta}</math>

<math>~=</math>

<math>~\frac{\partial}{\partial \theta}\biggl(\frac{GM}{r}\biggr) + \omega^2 r^2 \sin\theta \cos\theta \, .</math>

As presented in their equation (4.4), imposing the condition of uniform specific angular momentum leads to an angular velocity profile of the form,

<math>~\omega = \frac{\ell}{r^2 \sin^2\theta} \, .</math>


Comparison

Key References




Related Wikipedia Discussions


Whitworth's (1981) Isothermal Free-Energy Surface

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Recommended citation:   Tohline, Joel E. (2021), The Structure, Stability, & Dynamics of Self-Gravitating Fluids, a (MediaWiki-based) Vistrails.org publication, https://www.vistrails.org/index.php/User:Tohline/citation