## 3. The equation of transferThe key element and starting point in our research is a realistic expression for the differential Compton scattering cross section , describing scattering by electrons in relativistic thermal motion. In this research we adopted formulae from Guilbert (1981). The differential cross section can be decomposed according to where variable denotes the total
Compton scattering cross section (in cm In the following equations we shall use the function , which is defined as the zeroth angular moment of (Pomraning 1973). We introduce auxiliary functions and , which are defined by Both functions and contain stimulated scattering correction factors, and fulfil strictly the detailed balancing condition in thermodynamic equilibrium (cf. Paper I). We assume the following time-independent equation of radiative transfer, suitable for planar geometry where we included both thermal and scattering emission. We assume here nongrey true absorption , and noncoherent Compton scattering opacity, , both taken for 1 gram. Absorption coefficient included already LTE stimulated emission. Dimensionless absorption . Variable denotes the mean intensity of external irradiation at the level , with Following the standard approach we compute zero ## 3.1. Radiative equilibriumThe constraint of radiative equilibrium implies on each depth level that where (cgs units). Taking derivative of the above equation, we obtain the alternative form of the equation of radiative equilibrium where . Functions , , and are computed at the unknown temperature , in which they fulfil strictly the constraint of radiative equilibrium. ## 3.2. Hydrostatic equilibriumThe total scalar pressure , and the gradient of gas pressure in hydrostatic equilibrium is given by see also Paper II for more details. ## 3.3. Temperature correctionsWe assume linear Taylor expansions where , variables Then, we immediately obtain linear temperature corrections The sum equals the total mean intensity of radiation on the level . New functions, and , are defined by Variables , or 2, denote partial derivatives of the redistribution functions with respect to temperature and where . In thermodynamic equilibrium (, and ) we must have . ## 3.4. The equation of transfer and boundary conditionsFollowing the standard procedure we combine Eqs. 8 - 9 and get Such an equation implicitly contains unknown temperature corrections . Eddington factors . The final form of the equation of transfer is The above linearized equation of transfer was solved in the actual model stellar atmosphere computations.
The surface factor , which is equal to in the initial Eddington approximation. The above upper boundary condition is just a relation between the surface mean intensity and the flux. Factors can be iterated to exact, frequency-dependent values simultaneously with variable Eddington factors (Mihalas 1978). Note, that the upper boundary condition, Eq. 23, is formally the same as for a nonilluminated atmosphere. This is because the external illumination was explicitly separated in the equation of transfer, Eq. 6.
Useful form of that condition and its derivation is given in the Appendix. ## 3.5. Computational detailsFull set of model atmosphere equations solved in this paper consists of discretized radiative transfer Eqs. (22), written on frequencies , supplemented by the equation of hydrostatic equilibrium (12), and the equation for new temperatures , with given by Eq. (16). The LTE equation of state for ideal gas, and expressions for monochromatic opacities close the whole system. Actual model computations were performed with the two numerical assumptions: - For simplicity, electron scattering cross section per one
particle has been set to Thomson value,
cm - To avoid convergence problems, two Compton scattering terms in the equation of transfer, were always computed with the mean intensity on each depth level taken from the initial Thomson scattering model atmosphere, as described in Paper II. This approximation was absolutely necessary to avoid divergence of temperature corrections. However, such a choice certainly introduces some systematic errors. During a given iteration, tables of both integrals were carefully
recomputed for each optical depth
and running frequency , with new
temperatures determined at the end of previous iteration. Therefore
Compton scattering contribution to the equation of transfer was a
scalar inhomogeneity changing from one iteration to other, which was
just added to the thermal term (Planck function). The same applies to
scalars Method of solution and elimination scheme were adopted from Madej (1998), and Paper II, with the modifications described above. Convergence of our code was very rapid: in large part the redistribution of external hard X-ray flux to soft X-rays or EUV was computed in the first iteration. Relative temperature correction between neighbouring iterations were very large, and we had to artificially restrict them to max. 3-4, in order to avoid numerical instabilities. Computer code ATM21 represents implementation and extension of the partial linearization approach, described by Mihalas (1978, pp. 179-180). According to this, we did not linearize neither the variable , nor dimensionless absorption . We have neglected the effects of angular distribution of radiation in Compton scattering integrals just for simplicity. Also we have made other simplification by averaging of nonisotropic Compton scattering differential cross section over cosine of scattering angle, . However, it is necessary to point out here that Compton scattering of X-rays can be highly anisotropic, and then the significance of angular effects gets important. Hubeny (2000) expresses opinion, that for photon frequencies Hz (energies less than 40 keV) the angular effects may easily be more important than errors introduced by the Kompaneets equation approximation (which was rejected in this research). © European Southern Observatory (ESO) 2000 Online publication: December 5, 2000 |