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International Journal of Mathematics and Mathematical Sciences
Volume 2015 (2015), Article ID 479267, 11 pages
Research Article

Solving the Linear 1D Thermoelasticity Equations with Pure Delay

1Department of Cybernetics, Kyiv National Taras Shevchenko University, 64 Volodymyrska Street, Kyiv 01601, Ukraine
2Department of Mathematics and Statistics, University of Konstanz, Universitätsstraße 10, 78457 Konstanz, Germany

Received 27 October 2014; Accepted 3 January 2015

Academic Editor: Harvinder S. Sidhu

Copyright © 2015 Denys Ya. Khusainov and Michael Pokojovy. This is an open access article distributed under the Creative Commons Attribution License, which permits unrestricted use, distribution, and reproduction in any medium, provided the original work is properly cited.


We propose a system of partial differential equations with a single constant delay describing the behavior of a one-dimensional thermoelastic solid occupying a bounded interval of . For an initial-boundary value problem associated with this system, we prove a well-posedness result in a certain topology under appropriate regularity conditions on the data. Further, we show the solution of our delayed model to converge to the solution of the classical equations of thermoelasticity as . Finally, we deduce an explicit solution representation for the delay problem.

1. Introduction

Over the past half-century, the equations of thermoelasticity have drawn a lot of attention from the side of both mathematical and physical communities. Starting with the late 50s and early 60s of the last century, the necessity of a rational physical description for elastic deformations of solid bodies accompanied by thermal stresses motivated the more prominent mathematicians, physicists, and engineers to focus on this problem (see, e.g., [1, 2]). As a consequence, many theories emerged, mainly in the cross-section of (nonlinear) field theory and thermodynamics, making it possible for the equations of thermoelasticity to be interpreted as an anelastic modification of the equations of elasticity (cf. [3] and the references therein). Both linear and nonlinear models and solution theories were proposed.

An initial-boundary value problem for the general linear equations of classical thermoelasticity in a bounded smooth domain was studied by Dafermos in [4]. Here, and denote the (unknown) displacement vector field and the absolute temperature, respectively. Further, is the material density, is a reference temperature rendering the body free of thermal stresses, is the specific heat capacity, stands for Hooke’s tensor, is the stress-temperature tensor, is the heat conductivity tensor, represents the specific external body force, and is the external heat supply. Under usual initial conditions, appropriate normalization conditions to rule out the rigid motion as a trivial solution, and general boundary conditions where are relatively open, denotes the “elasticity” modulus, and is heat transfer coefficient, Dafermos proved the global existence and uniqueness of finite energy solutions and studied their regularity as well as asymptotics as . In 1D, even an exponential stability result for (1)-(2) under all “reasonable” boundary conditions was shown by Hansen in [5].

In his work [6], Slemrod studied the nonlinear equations of 1D thermoelasticity in the Lagrangian coordinates for the unknown functions denoting the displacement of the rod and being a temperature difference to a reference temperature rendering the body free of thermal stresses. The functions and denote the Helmholtz free energy and the heat flux, respectively, and are assumed to be given. Finally, is the material density in the references configuration. Under appropriate boundary conditions (when the boundary is free of tractions and is held at a constant temperature or when the body is rigidly clamped and thermally insulated) as well as usual initial conditions for both unknown functions, a local existence theorem for (4) was proved by additionally imposing a regularity and compatibility condition. For sufficiently small initial data, the local classical solution could be globally continued. At the same time, when studying (4) in the whole space, large data are known to lead to a blow-up in final time (cf. [7]).

Racke and Shibata studied in [8] (4) under homogeneous Dirichlet boundary conditions for both and . Under appropriate smoothness assumptions, they proved the global existence and exponential stability for the classical solutions to the problem. In contrast to Slemrod [6], their method was using spectral analysis rather than ad hoc energy estimates obtained by differentiating the equations with respect to and . A detailed overview of further recent developments in the field of classical thermoelasticity and corresponding references can be found in the monograph [9] by Jiang and Racke.

The classical equations of thermoelasticity outlined above, being a hyperbolic-parabolic system, provide a rather good macroscopic description in many real-world applications. At the same time, they sometimes fail when being used to model thermoelastic stresses in some other situations, in particular, in extremely small bodies exposed to heat pulses of large amplitude (see, e.g., [10]) and so forth. To address these issues, a new theory, commonly referred to as the theory of hyperbolic thermoelasticity or second sound thermoelasticity, has emerged. In contrast to the classical thermoelasticity, parabolic equation (2) is replaced with a hyperbolic first-order system with and denoting the heat flux and the relaxation tensor, respectively. Both linear and nonlinear versions of the equations of hyperbolic thermoelasticity (1), (5)-(6) have been studied in the literature. See, for example, [11] by Messaoudi and Said-Houari for a proof of global well-posedness of the 1D system in the whole space or Irmscher’s work [12] for the global well-posedness of nonlinear problem for rotationally symmetric data in a bounded rotationally symmetric domain of . In a bounded 1D domain, a quantitative stability comparison between the classical and the hyperbolic system was presented by Irmscher and Racke in [13]. For a detailed overview on hyperbolic thermoelasticity, we refer the reader to [14] by Chandrasekharaiah and [15] by Racke.

A unified approach establishing a connection between the classical and hyperbolic thermoelasticity was developed by Tzou in [16, 17]. Namely, he proposed to view (6) with as a first-order Taylor approximation of the equation being equivalent to the delay equation More generally, higher-order Taylor expansion to the dual phase lag constitutive equation can be considered. Together with (1)-(2), (5), this leads to the so-called dual phase lag thermoelasticity studied by Racke (cf. references in [15, page 415]).

If no Taylor expansion with respect to is carried out in (8), it can be shown that the corresponding system is ill-posed when being considered in the same topology as the original system of classical thermoelasticity (cf. [18]); that is, the system is lacking a continuous dependence of solution on the data. Moreover, the delay law (8) can, in general, contradict the second law of thermodynamics as shown in [19].

Nonetheless, it remains desirable to understand the dynamics of equations of thermoelasticity originated from delayed material laws. One of the first attempts to obtain a well-posedness result for a partial differential equation with pure delay is due to Rodrigues et al. In their paper [20], Rodrigues et al. studied a heat equation with pure delay in an appropriate Frechét space and showed the delayed Laplacian to generate a -semigroup on this space. Further, they investigated the spectrum of the infinitesimal generator. Though their approach can essentially be carried over to the equations of thermoelasticity with pure delay derived in Section 2, we propose a new approach in this paper preserving the Hilbert space structure of the space and thus the connection to the classical equations of thermoelasticity. To the authors’ best knowledge, no results on thermoelasticity with delay in the highest order terms have been previously published in the literature. At the same time, we refer the reader to the works by Khusainov et al. [2124], in which the authors studied the well-posedness and controllability for the heat and/or the wave equation on a finite time horizon. In their recent paper [25], Khusainov et al. exploited the -maximum regularity theory to prove a global well-posedness and asymptotic stability results for a regularized heat equation with delay.

The present paper has the following outline. In Section 2, we give a physical model for linear thermoelasticity based on delayed material laws. For the sake of simplicity, we present a 1D model though our approach can easily be carried over to the general multidimensional case. Next, in Section 3, we prove the well-posedness of this model in an appropriate Hilbert space framework and discuss the small parameter asymptotics, that is, the behavior of solutions as . Further, in Section 4, we deduce an explicit solution representation formula. Finally, in the Appendix, we summarize some seminal results on the delayed exponential function and Cauchy problems with pure delay.

2. Model Description

We consider a solid body occupying an axis-aligned rectangular domain of . Assuming that the body motion is purely longitudinal with respect to the first space variable (cf. [6, page 100]), deformation gradient, stress and strain tensors, and so forth are diagonal matrices and a complete rational description of the original 3D body motion can be reduced to studying the 1D projection , , of the body onto the -axis as displayed in Figure 1. Hence, in the following, we restrict ourselves to considering the relevant physical values only in -direction.

Figure 1: 3D rectangular solid body.

Let the functions and denote the body displacement and its relative temperature measured with respect to a reference temperature rendering the body free of thermal stresses, respectively. We restrict ourselves to the Lagrangian coordinates and write for the stress field, strain field, entropy field, or the heat flux, respectively. With denoting the material density, the momentum conservation law as well as the linearized entropy balance law reads as where and are a known volume force acting on the body and an internal heat source.

Assuming physical linearity for the strain field, the strain can be decomposed into elastic strain and thermal stress . Further, assuming uniformly with respect to , , we can postulate where denotes the thermal expansion coefficient. Exploiting the second law of thermodynamics for irreversible processes, we obtain (cf. [3, page 3]) with standing for the specific heat capacity and denoting the bulk modulus.

In our further considerations, we depart from the classical material laws and use their delay counterparts. Let be a positive time delay. In the sequel, all functions are supposed to be defined on . Assuming a delay feedback between the stress and the strain as well as the heat flux and the temperature gradient, Hooke’s law with pure delay reads as (cf. [1]) with denoting the shear modulus. Similarly, we consider a delay version of Fourier’s law given as where stands for the thermal conductivity. Assuming the elastic strain tensor to be equal to the displacement gradient, we have We further postulate the following relation: which is a delayed counterpart of Schwarz’s theorem. Finally, we also modify (12) to introduce a delay feedback between the entropy, the elastic strain tensor, and the temperature Exploiting now (10), (13)–(17), we obtain To close (18), appropriate boundary and initial conditions for and are required. In the following, we prescribe homogeneous Dirichlet boundary conditions for and homogeneous Neumann boundary conditions for given as This particular choice of boundary conditions not only turns out to be convenient for our further mathematical considerations but also is a physically relevant one. Similar to the thermoelasticity with second sound, it is one of the combinations typically arising when studying micro- and nanoscopic strings or plates (cf. [13]).

The initial conditions are given over the whole history period and read as with known and .

3. Well-Posedness and Limit

Letting , , , and , and for , , (18) can be rewritten as subject to the boundary conditions from (19) and initial conditions from (20). Introducing a new vector of unknown functions, Equations (21) can be transformed to with the differential matrix operator and the right-hand side respectively.

Exploiting (19) and the definition of , the boundary conditions for read as whereas the initial conditions are given by with Note that (18)–(20), (23), (25), and (26) are equivalent for; if the vector is known, and are uniquely determined by Therefore, in the sequel, we consider the following equivalent first-order-in-time problem: For our well-posedness investigations, we need a solution notion for (29). To this end, appropriate functional spaces have to be introduced. We start with the “naïve” approach by using the case as a reference situation. We introduce the Hilbert space equipped with the dot product and define the operator with the domain See [26, Section 3] for the definition of Sobolev spaces. With this notation, (29) can be written in the equivalent form Under a classical solution to (33) on for any , one would naturally understand a function satisfying the equations pointwise.

We know from [5] that the linear operator is accretive and satisfies . Its spectrum only consists of isolated eigenvalues , , of finite multiplicity with , , and as . The corresponding eigenfunctions build an orthonormal basis of . Unfortunately, from [18, Theorem 1.1] we know that (33) is ill-posed in . Hence, a different solution notion should be adopted. As we already mentioned in Section 1, we want to preserve the Hilbert space structure of the problem and thus cannot follow the approach developed by Rodrigues et al. in [20].

For , we define the space equipped with the scalar product induced by the norm Hence, is closed subspace of and thus a Hilbert space. Moreover, is dense in since . Indeed, for , we have and .

Restricting to the closed subspace of , we trivially obtain a bounded linear operator since for Now, restricting (33) to , we obtain Following the approach in [21], we introduce for the delayed exponential function Figure 2 displays the delayed exponential function for the case where is a real number.

Figure 2: Delayed exponential function.

Obviously, for any , . Moreover, we have uniformly in since Here, denotes the space of bounded, linear operators from to equipped with the standard operator topology.

Now, we can prove the following well-posedness result.

Theorem 1. For , let , with and let . Then (36) possess a unique classical solution explicitly given by

Proof. First, we prove uniqueness of classical solutions. Assuming and to be classical solutions of (36), we conclude that their difference is a classical solution to Multiplying these equations with in the inner product of , we further deduce that , , is a classical solution to the scalar delay differential equation From Theorem A.4 in the Appendix, the later equations are known to be uniquely solvable by . Hence, for all . With being a basis of , this implies , and, therefore, .
For the existence proof, we show that the function in (40) is a classical solution to (36). Performing the diagonalization, we obtain for From [25], we know for all . Further, by the virtue of (38), the series converges uniformly in and its derivative converges uniformly in . Hence, the limiting function lies in and thus possesses the regularity of a classical solution. Finally, using the properties of scalar delay exponential (cf. [25]), we easily verify that solves (36).

Taking into account inequality (38) and applying Hölder’s inequality to (40), we obtain the following estimate.

Corollary 2. The solution continuously depends on the data in sense of the estimate

For the rest of this section, we want to study the behavior of system (33) as . Let and be fixed. Similar to , we consider the Hilbert space equipped with the scalar product induced by the norm Obviously, . For simplicity, despite a slight abuse of notation, we let now denote the part of in (namely, [27, page 139]). Formally, the limiting system of (33) as is given by From [27, Corollary 3.3.13], we know that generates a uniformly bounded -semigroup of bounded linear operators on . The unique classical solution to (46) can then be written using Duhamel’s formula as Theorem A.3 from the Appendix implies the following.

Lemma 3. There holds

Now, we can prove the following.

Theorem 4. Let , be fixed. For , let with and . Denoting with the classical solution of (36) corresponding to the initial data , and the right-hand side , one has

Proof. Using the representation formulas for and , we can estimate for any This finishes the proof.

4. Explicit Solution Representation

In this section, we want to deduce an explicit representation of solutions to (36) in the form of a Fourier series with respect to an orthogonal basis of (and thus of ) given by with Note that the sequence does not coincide, in general, with the eigenfunctions but, at the same time, constitutes a basis of . To this end, we assume that the conditions of Theorem 1 are satisfied which yields a unique classical solution .

Denoting and computing the componentwise Fourier coefficients for and , we get the following Fourier expansions: uniformly in (due to the Sobolev embedding theorem). Similarly, the solution can be expanded into Fourier series for some , , , to be determined later. Using this ansatz and letting we observe that (36) decompose into a sequence of ordinary delay differential equations By the virtue of Theorem A.4, for any , the unique solution to (57) is given by To explicitly compute the function given in (58), we need to diagonalize the matrix .

Lemma 5. Let where and   stand for the main branch of complex square and cubic roots. The spectrum of   consists of three eigenvalues for with denoting the imaginary unit.

Proof. For , we have and therefore . Hence, is the only eigenvalue of   with an algebraic multiplicity of .
Now, let us assume . To compute the eigenvalues of , we consider the characteristic polynomial Since the matrix has real components and is skew-symmetrizable, it has to possess one real and two complex-conjugate eigenvalues. Thus, introducing the expressions we obtain the three roots , , of (cf. [28, page 179]) where and   stand for the main branch of complex square and cubic roots.

Lemma 6. Eigenvectors , , of corresponding to the eigenvalues of from Lemma 5 are given by with , , and .

Proof. Since the first case is obvious, we only consider the case . For , we consider the matrix The latter is singular since is an eigenvalue of . Further, due to the fact that is invertible and, therefore, . We want to find a nontrivial vector satisfying Thus, we can apply a Gauss-Jordan iteration to the former matrix and find Since the latter matrix must be singular, the third row must be proportional to the second one. Thus, (68) is equivalent to Since the rank of this matrix is 2, the equation above yields only one eigenvector being determined up to a multiplicative constant.

Note that , , and are linearly independent, but, in general, not orthonormal.

Letting now we obtain a singular value decomposition for with an invertible matrix Exploiting now Corollary A.2 from Appendix, (58) can finally be written as where the inverse of is given by the Laplace formula


Ordinary Delay Differential Equations

Let be a (real or complex) Hilbert space and let be arbitrary. For a bounded linear operator on , we consider the following ordinary delay differential equation: for some , , and .

Since the delay exponential function is an operator polynomial in piecewise with respect to , we obviously have the following representation.

Theorem A.1. Let be an isomorphism. Then

Corollary A.2. If , , and is diagonalizable over , that is, if there exists a diagonal matrix , , and an invertible such that , then

Theorem A.3. Let , , and and let . Then, for any ,

Proof. Let . For , the claim immediately follows from the mean value theorem for integration. We use mathematical induction to prove for any Indeed, assuming that the claim is true for some , the fundamental theorem of calculus yields for as . Finally, the claim follows by induction.

According to [25, Theorem 3.12], we have the following well-posedness result for (A.1).

Theorem A.4. The delay differential equation (A.1) possesses a unique strong solution given by If lies in and satisfies the compatibility condition , then the strong solution is even a classical solution; that is, .

Conflict of Interests

The authors declare that there is no conflict of interests regarding the publication of this paper.


The investigations were supported by the Young Scholar Fund (Research Grant ZUK 52/2 of the Deutsche Forschungsgemeinschaft) at the University of Konstanz, Konstanz, Germany. The authors express their deep gratitude to the anonymous referee for the careful reading of the paper and the valuable comments and suggestions.


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