Research Article | Open Access
Maria Cristina Carrisi, Rita Enoh Tchame, Marcel Obounou, Sebastiano Pennisi, "A Numberable Set of Exact Solutions for the Macroscopic Approach to Extended Thermodynamics of Polyatomic Gases with Many Moments", Advances in Mathematical Physics, vol. 2016, Article ID 1307813, 8 pages, 2016. https://doi.org/10.1155/2016/1307813
A Numberable Set of Exact Solutions for the Macroscopic Approach to Extended Thermodynamics of Polyatomic Gases with Many Moments
A new model for Polyatomic Gases with an arbitrary but fixed number of moments has been recently proposed and investigated in the framework of Extended Thermodynamics; the arbitrariness of the number of moments is linked to a number and the resulting model is called an -Model. This model has been elaborated in order to take into account the entropy principle, the Galilean relativity principle, and some symmetry conditions. It has been proved that the solution for all these conditions exists, but it has not been written explicitly because hard notation is necessary; it has only been shown how the theory is self-generating in the sense that if we know the closure of the -Model, then we will be able to find that of -Model. Up to now only a single particular solution has been found in this regard. Instead of this, we find here a numberable set of exact solutions which hold for every fixed number .
The model for Polyatomic Gases considers for every number the following balance equations:and the resulting model is called an -Model.
Here represents the momentum-like hierarchy, while represents the energy-like hierarchy; the quantities with an index represent their fluxes, while and represent the production terms; for the conservation laws of mass and momentum we have and , while for the conservation of energy we have .
This model represents a novelty with respect to the earlier versions of Extended Thermodynamics (ET) which used only (1)1 obtaining the important result to have a symmetric hyperbolic system of partial differential equations, with finite speed of propagation of shock waves and other important properties. A very short list of significative articles in this regard is given in [1–7]. These results constituted an important improvement of the models of Ordinary Thermodynamics. A very significative article in this previous framework is given in . But ET was still not completely satisfactory because it is too much restrictive also on the state function relating the pressure to the mass density and energy density . This problem has been overcome in Extended Thermodynamics of Polyatomic Gases by considering all the balance equations (1) of which the first one is called the “Mass-Block” of equations and the second is called the “Energy-Block” of equations. See, for example, the articles [9–16].
It has to be noted that in the literature here cited the balance equations are not included in the -Model, but they can be easily recovered with the theory of subsystems (see ) by simply putting the Lagrange multiplier of the last equation in the Mass-Block equal to zero. In [11, 12] it has been shown that the wave speeds of the -Model are the same as those of monatomic gases; but this proof has been given with the kinetic equations which are only a subcase of those of the macroscopic approach (in effect, the whole closure here found is zero in the kinetic approach and only parts (5) and (6) remains). In any case there is no problem for what we have said at the beginning of this note. Moreover, a priori the Bhatnagar-Gross-Krook equation (see the equation before in ) can be replaced by an infinite hierarchy of balance equations for moments and only for practical reasons some of them are eliminated; consequently, there is no inconsistence if another of these balance equations is eliminated in a second step with the theory of subsystems, as said above. The -Model is here considered because it makes (in the macroscopic approach) the decomposition of tensors in nonconvective parts and in velocity dependent parts more linear. In the kinetic approach this is simply a consequence of the integrals, but in the macroscopic approach here followed this decomposition must be justified in a straightforward manner. In [11, 12] the -system has been proposed with ; but the macroscopic approach needs a much heavier notation and this is simplified by the present -Model without losing generality because, in any case, the -system can be recovered from the present one with the theory of subsystems.
In (1) the independent variables are and ; the quantities and are their corresponding fluxes. The problem will be closed when we know the expressions of and as functions of the independent variables. Restrictions on their generality are obtained by imposing the entropy principle, the Galilean relativity principle, and the symmetry conditions. These last ones express the fact that each flux in (1) is equal to the independent variable of the subsequent equation, except for the flux in the last equation of the Mass-Block and for that in the last equation of the Energy-Block; for these last fluxes we know only that they are symmetric tensors.
The Entropy Principle, exploited through Liu’s Theorem  and a bright idea conceived by Ruggeri and Strumia , becomes equivalent to assuming the existence of Lagrange Multipliers and which can be taken as independent variables and, after that, we havewhich expresses all the moments in terms of only two unknown functions, the 4-potential and . Their relation with the entropy and its flux is given by A nice consequence of (2) is that the field equations assume the symmetric form. Another consequence of (2) is that the above-mentioned symmetry conditions and the Galilean relativity principle can be expressed asThe equivalence of (4)5 to the Galilean relativity principle is proved in literature such as [13, 20, 21] and on Representation Theorems such as that of .
In (5), (6), and (7) we report an already known particular solution (see ) for the conditions (4). But it is not the general solution; in fact, in the present article we will exhibit a significative set of other solutions depending on a numberable family of arbitrary single variable functions and we report it in the next section, (8) and (9). It is expressed through Taylor’s expansion around equilibrium which is defined as the state where , for , and , for , so that the only variables which are not zero at equilibrium are and . The first of these is the chemical potential, while with absolute temperature.
Obviously, also the velocity is nonvanishing at equilibrium; but if we use a decomposition in nonconvective parts and in velocity dependent parts, we obtain the Lagrange multiplier of the momentum conservation law in terms of the other Lagrange multipliers and we see that its velocity independent part is zero at equilibrium. Moreover, from the fact that the velocity independent parts of and are zero at equilibrium, it follows that they are zero also as a whole, without decomposition; the only exceptions are for the Lagrange multipliers of the mass and of the energy conservation laws (see equation of , e.g.).
2. A Set of Exact Solutions for Conditions (4)
Before writing our solution we need an apparently complicated notation.
To do the derivatives with respect to a number of times, we use the compact form to indicate a set of indexes, to indicate another set of indexes, and so on up to , so that the first index of indicates how many indexes have the corresponding , while the second index of indicates how many derivatives we are taking with respect to it. Similarly, to do the derivatives with respect to a number of times, we use the compact form to indicate a set of indexes, to indicate another set of indexes, and so on up to . After describing this notation, we can now report from  the already known solution for our conditions and it iswhere is a family of functions depending only on and and constrained only byBut the above one is not the unique solution; in fact, by using the same notation, we can now say that a more general solution can be obtained by adding to (5) and (6) the following expressions (8) and (9); that is,where is a family of functions depending only on such that for . Here we use only a letter as a shortened symbol denoting the product of some each one with 2 indexes and with a final symmetrization over all these indexes.
We note the following:(i)If , the function in the expression of has index and consequently this may be different from zero only if and ; but in this case is not odd. This fact implies that . Similarly, the function in the expression of has index so that and . This confirms the results of  for this case , because in the sum of (8) and (9) and the corresponding results (5) and (6) of  only these last ones remain in the case .(ii)If , the function in the expression of has index and this is an odd number because must be odd. Consequently, the index belongs to the interval if this is not the empty set. By taking into account this fact we see that the sum of the solution reported in (6) and the present expression (9) for the case is the same as that in . Similarly, the function in the expression of has index and this is an odd number because must be even. Consequently, the index belongs to the interval if this is not the empty set. By taking into account this fact we see that the sum of our expression (8) and that in (5) for the case is the same as that in .(iii)If our solution is completely new.
In this section we prove that (8) and (9) are a solution for (4)1–4, putting off (4)5 to Section 4:(i)Let us substitute firstly (8) and (9) in (4)1. We obtain for both sides the following expression: where we have taken into account that here is denoted with or with and so on up to . Similarly, is denoted with or with and so on up to . Consequently, the left hand side of (4)1 causes, with respect to expression (9), a rise of one unity of the index ; similarly, the right hand side of (4)1 causes, with respect to expression (8), a rise of one unity of the index .(ii)It is easy to verify that (9) satisfies (4)2,4.(iii)By substituting (8) and (9) in (4)3 in the case , we obtain for both sides the following expression: where we have taken into account that here is denoted with or with and so on up to . Similarly, is denoted with or with and so on up to . Consequently, the left hand side of (4)3 with causes, with respect to expression (9), a rise of one unity of the index ; similarly, the right hand side of (4)3 with causes, with respect to expression (8), a rise of one unity of the index .(iv)Let us conclude substituting (8) and (9) into (4)3 in the case . We have the same situation of the above case for its right hand side, while for its left hand side we have to take simply the derivative of (9) with respect to . More precisely, we obtain for both sides the following expression:This concludes our proof that (4)1–4 are satisfied by (8) and (9). In the next section we will consider (4)5.
First of all we note that (4)5 can be rewritten as
(i) After that, we note that the first term of this relation thanks to (8) becomes because the derivation causes a presence of the factor and the substitution of with and the new free indexes in the expression of ; moreover, we have also substituted with . Now in the resulting expression we can insert a symmetrization over all the indexes of the set because that expression remains the same if we exchange two of these indexes. This fact is evident if the two indexes are taken between ; for the proof in the other cases, let us consider the shortened expression ; here we can exchange the names of the indexes with those of , so that the above shortened expression becomes .
Now we can exchange the indexes with the indexes in the expression of because this is a symmetric tensor.
We obtain . By comparing this result with the expression which we started from, it is the same if we had exchanged the indexes and . This completes the proof of the fact that expression (14) remains the same if we exchange two indexes of the set ; so we can insert there a symmetrization over those indexes and (14) becomeswhere underlined indexes denote symmetrization over these indexes. Now we observe that is exactly the number of the indexes of the set and that, thanks to the summation , the index near in can be every index of the set . These facts allow rewriting (15) as
(ii) For the fourth term of (13) we can do similar passages (the difference is that we have instead of , instead of , and instead of ); in this way that term becomes
(iii) If we look at the last term of (13), we see that it can be written together with (16) and (17) and they become where also the index has been put under the symmetrization and we recall that a property of symmetrization is . We note that the coefficient in square bracket at the beginning of the right hand side of (18) has become equal to the denominator of the half factorial of that right hand side.
(v) There remains considering the third term of (13); for it we can use (8) and the derivation causes someway the rising of one unity of the index ; in this way it becomes In this expression, we can substitute with and with ; moreover, we substitute with and, after that, decrease of one unity (which is equivalent to a change of index). So this expression becomesIt is true that with change of index we have in the summation the extra term with ; but it does not effect the result for the presence of the coefficient .