2.1 Conservation of fluxes and the form Q

During the entire approach, we will work with a number $l\in \mathbb{N}$ that gives the width of a so called ‘radiation box’. The number is arbitrary, but fixed throughout this article; accordingly, we nowhere mark the dependence of l by a sub- or superscript. The reader might want to think of $l=1$ in the whole text. Given $l>0$ , we consider the central box $W_0 := (0,l) \times S$ and, for arbitrary $r\in \mathbb{Z}$ , the shifted boxes $W_r := (r,r+l)\times S$ .

We describe the situation first for a periodic medium a. We can identify a function $u: W_r \to \mathbb{C}$ with the function $\tilde u:W_0\to \mathbb{C}$ , which is obtained with a shift: $\tilde u(x) := u(x+r e_1)$ .

Of crucial importance in our approach will be the following sesquilinear form Q. For $u\in H^1(W_0)$ and $v\in L^2(W_0)$ , we define

(2.1) \begin{equation} Q(u,v) := \frac1{l} \int_{W_0} a\nabla u \cdot e_1 \bar v\,,\quad \text{ and }\quad \mathcal{Q}(u) := Q(u,u)\,,\end{equation}

where the overbar denotes complex conjugation. The sesquilinear form Q and the quadratic form $\mathcal{Q}$ are used to measure the energy flux of solutions. We also consider an (anti-)symmetrised variant of Q,

(2.2) \begin{equation} Q^s(u,v) := \frac1{2} \left( Q(u,v) - \overline{Q(v,u)} \right)\,.\end{equation}

The symmetrised variant satisfies $Q^s(u,v) = - \overline{Q^s(v,u)}$ and $Q^s(u,u) = i\, \mathrm{Im}\, \mathcal{Q}(u)$ . We mention already here that a more standard description of the flux $\mathrm{Im}\, \mathcal{Q}(u)$ as a surface integral is given with formula (2.5) of Remark 2.2 below.

We will repeatedly use piecewise affine cut-off functions $\vartheta$ that are 1 in an interior interval and 0 outside a larger interval. More precisely, given four consecutive points $(\rho, \rho + l, r, r+l)$ , we set: $\vartheta(s) = 0$ for $s\le \rho$ and for $s\ge r+l$ , $\vartheta(s) = 1$ for $\rho +l \le s \le r$ , and $\vartheta$ affine linear in the two remaining intervals, compare Figure 3. By slight abuse of notation, we identify $\vartheta$ with a cut-off function on $\Omega$ by setting $\vartheta(x) := \vartheta(x_1)$ for $x\in \Omega$ .

Figure 3.

The cut-off function $\vartheta$ .

The basis for our approach is the energy flux equality. In its simplest form, it states: For a homogeneous solution $\phi$ , the energy flux quantity $\mathrm{Im}\, \mathcal{Q}(\phi|_{W_r})$ is independent of the position r. We use the notation $\Omega_{r_1, r_2} := (r_1, r_2) \times S$ .

Lemma 2.1 (Simple flux equality) Let $\phi, \psi\in H^1_\mathrm{loc}(\Omega)$ be two solutions to $A\phi = \omega^2 \phi$ on $\Omega$ . Then, for arbitrary $\rho, r\in \mathbb{R}$ with $\rho + l \le r$ , there holds the flux equality

(2.3) \begin{equation} \mathrm{Im}\, \mathcal{Q}(\phi|_{W_\rho}) = \mathrm{Im}\, \mathcal{Q}(\phi|_{W_r})\,. \end{equation}

The sesquilinear form $Q^s$ satisfies

(2.4) \begin{equation} Q^s(\phi|_{W_\rho}, \psi|_{W_\rho}) = Q^s(\phi|_{W_r}, \psi|_{W_r})\,. \end{equation}

Proof. Equality (2.4) implies (2.3) by $Q^s(u,u) = i\, \mathrm{Im}\, \mathcal{Q}(u)$ .

We use the piecewise affine cut-off function $\vartheta$ corresponding to the four points $(\rho, \rho + l, r, r+l)$ . Multiplication of the equation $A\phi = \omega^2 \phi$ with $\vartheta \bar\psi$ and an integration over $\Omega$ yields

\begin{align*} 0 &= \int_{\Omega_{\rho, r+l}} a\nabla \phi\cdot \nabla (\bar \psi \vartheta) - \int_{\Omega_{\rho, r+l}} \omega^2\, \phi\, \bar \psi\, \vartheta\\[3pt] &= \int_{\Omega_{\rho, r+l}} a\nabla \phi\cdot \nabla \bar \psi\, \vartheta - \int_{\Omega_{\rho, r+l}} \omega^2\, \phi\, \bar \psi\, \vartheta - \int_{W_r} a\nabla \phi\, \bar \psi\cdot \frac1{l} e_1 + \int_{W_\rho} a\nabla \phi\, \bar \psi\cdot \frac1{l} e_1\\[3pt] &= \int_{\Omega_{\rho, r+l}} a\nabla \phi \cdot \nabla \bar\psi\, \vartheta - \int_{\Omega_{\rho, r+l}} \omega^2\, \phi\, \bar\psi\, \vartheta - Q(\phi|_{W_r}, \psi|_{W_r}) + Q(\phi|_{W_\rho}, \psi|_{W_\rho})\,. \end{align*}

The same expression can be written with $\phi$ and $\psi$ exchanged; performing additionally a complex conjugation, we have

\begin{align*} 0 &= \int_{\Omega_{\rho, r+l}} a\nabla \phi \cdot \nabla \bar\psi\, \vartheta - \int_{\Omega_{\rho, r+l}} \omega^2\, \phi\, \bar\psi\, \vartheta - \overline{Q(\psi|_{W_r}, \phi|_{W_r})} + \overline{Q(\psi|_{W_\rho}, \phi|_{W_\rho})}\,. \end{align*}

Subtracting the two results, the first two integrals cancel and we obtain (2.4).

Remark 2.2 (The flux through an interface). Let $\phi\in H^1_\mathrm{loc}(\Omega)$ be a solution of $A\phi = \omega^2 \phi$ on $\Omega$ . Multiplication with $\bar\phi$ , integration over $(\rho, r)\times S \subset \Omega$ and taking the imaginary part yields

(2.5) \begin{equation} \mathrm{Im}\, \int_{\{ \rho \} \times S} a\nabla\phi\cdot e_1\ \bar\phi = \mathrm{Im}\, \int_{\{ r \} \times S} a\nabla\phi\cdot e_1\ \bar\phi \end{equation}

in the sense of traces. This shows that the expression on the right does not depend on the position r.

The fact that the surface integral is independent of r implies that every volume integral $\mathrm{Im}\, \mathcal{Q}(\phi|_{W_r})$ of (2.3) actually coincides with the expression in (2.5).

2.2 Propagating modes and radiation condition

We next study solutions to the radiation problem. We are interested in solutions u that do not decay at infinity. Regarding regularity, on the other hand, we cannot expect that solutions are locally of class $L^\infty$ . We therefore introduce a new norm to measure functions. For $u:\Omega\to \mathbb{C}$ we set

(2.6) \begin{equation} \| u \|_{sL} := \sup_{r\in \mathbb{Z}} \| u \|_{L^2((r,r+1)\times S)}\,.\end{equation}

We have chosen the subscript sL for the norm to recall that a supremum over $L^2$ -norms is taken. We study the following subspace of $H^1(W_0)$ :

(2.7) \begin{equation} X := \left\{ u|_{W_0}\, \middle| \, u\in H^1_\mathrm{loc}(\Omega),\ \| u \|_{sL} < \infty,\ Au = \omega^2 u \text{ in } \Omega \right\}\,.\end{equation}

In many situations (see the text below), it is known that all functions u in (2.7) are quasiperiodic functions. We say that a function $u : \Omega\to \mathbb{C}$ is quasiperiodic if there exists a real number $\xi\in [0, 2\pi)$ such that $u(x+e_1) = e^{i\xi} u(x)$ for every $x\in \Omega$ . The number $\xi$ is called the quasimoment and we also say that u is $\xi$ -quasiperiodic. Note that, when u is $\xi$ -quasiperiodic, u can be reconstructed from $u|_{W_0}$ .

Let us recall some spectral analysis facts. In the next paragraph, we describe a generic situation and typical methods. We do not cite the rigorous mathematical results. Our intention is rather to clarify that the assumptions in our main theorems are reasonable. The proofs of our theorems do not use any of the results sketched here. For more material on the spectral analysis, we refer to [Reference Fliss and Joly9, Reference Kuchment16, Reference Kuchment17, Reference Reed and Simon21].

For a fixed number $\xi\in [0, 2\pi),$ one can consider the space of all $\xi$ -quasiperiodic functions v. The Floquet-Bloch transform allows to decompose the partial differential equation $Au = \omega^2 u$ into a family of problems $A(\xi) u = \omega^2 u$ , where $\xi\in [0, 2\pi)$ is the quasimoment and $A(\xi)$ is the operator A restricted to $\xi$ -quasiperiodic functions. Every operator $A(\xi)$ has a compact resolvent and hence a pure point spectrum. The eigenvalues of $A(\xi)$ depend continuously on $\xi$ and have lower bounds which imply that, for generic values of $\omega$ , the number $\omega^2$ coincides with eigenvalues of $A(\xi)$ only for finitely many values of $\xi$ . The corresponding finitely many eigenfunctions then form a basis of the space X of (2.7). In particular, the space X is finite-dimensional.

We will assume this situation and one additional property: For the frequency $\omega$ , the imaginary part of the form $\mathcal{Q}$ does not vanish in basis functions. If, for every $\xi$ , $\omega^2$ is not a multiple eigenvalue of $A(\xi)$ , then our definition of non-singular frequencies coincides with the one in [Reference Fliss and Joly9], see the set $\sigma_0$ in (33) of [Reference Fliss and Joly9]. We emphasise that our space X is, a priori, not identical with the space F of propagating Floquet modes; instead, X could be larger and we essentially say that a frequency is non-singular when no mode of X is propagating. It is an interesting task for future research to check under what conditions $X = F$ holds.

Whenever $\omega>0$ is a non-singular frequency, we can actually achieve the following situation: There holds $M = 2N$ for some $N\in \mathbb{N}$ , there exists a basis $(\phi_1^+, ... , \phi_{N}^+$ , $\phi_1^-, ... , \phi_{N}^-)$ of X and corresponding quasimoments $\xi_j^\pm\in [0,2\pi)$ such that the quasiperiodic extensions with $\phi_j^\pm(.+e_1) = e^{i \xi_j^\pm} \phi_j^\pm(.)$ solve $A \phi = \omega^2 \phi$ in $\Omega$ . For two basis functions $\phi$ and $\tilde\phi$ for the same quasimoment $\xi$ , there holds the orthogonality $Q^s(\phi, \tilde\phi) = 0$ . Furthermore, the fluxes have a sign as indicated by the superscript: For every j holds

(2.9) \begin{equation} \mathrm{Im}\, \mathcal{Q}(\phi_j^+) > 0\quad \text { and }\quad \mathrm{Im}\, \mathcal{Q}(\phi_j^-) < 0\,.\end{equation}

Let us indicate how to obtain the basis $(\phi_1^+, ... , \phi_{N}^+$ , $\phi_1^-, ... , \phi_{N}^-)$ . We fix a quasimoment $\xi$ and consider only the basis functions $\varphi_j$ having that quasimoment, say $\varphi_1, ..., \varphi_m$ . We perform a standard diagonalisation procedure with respect to $Q^s$ : In the first step, we choose $\phi_1 =\varphi_1$ . In the second step, we set $\alpha_1 = Q^s(\phi_1, \varphi_2)/Q^s(\phi_1, \phi_1)\in \mathbb{C}$ , which is possible by condition (b) and $Q^s(u,u) = i\, \mathrm{Im}\, \mathcal{Q}(u)$ , and define $\phi_2 = \varphi_2 - \alpha_1 \phi_1$ . This guarantees $Q^s(\phi_1, \phi_2) = Q^s(\phi_1, \varphi_2) - \alpha_1 Q^s(\phi_1,\phi_1) = 0$ . The (anti-)symmetry of $Q^s$ yields additionally $Q^s(\phi_2, \phi_1) = 0$ . The process can be continued until $\varphi_1, ..., \varphi_m$ are $Q^s$ -orthogonalised. We exploit in the process the symmetry of $Q^s$ and the fact that, for fixed $\xi\in \mathbb{R}$ , $\xi$ -quasiperiodic functions form a vector space. Relabelling the functions $\phi_1, ..., \phi_M$ and exploiting once more (b), we obtain (2.9).

Below, we will obtain additionally the orthogonality of all basis functions $\phi_j^\pm$ with respect to the form $Q^s$ . Given a function $\phi_j^+$ with $\mathrm{Im}\, \mathcal{Q}(\phi_j^+) > 0$ , the complex conjugate function $\overline{\phi_j^+}$ is also contained in the space X of (2.7), it satisfies $\mathcal{Q}(\overline{\phi_j^+}) = \overline{\mathcal{Q}(\phi_j^+)}$ and hence $\mathrm{Im}\, \mathcal{Q}(\overline{\phi_j^+}) < 0$ . This argument shows that the number of modes $\phi_j^+$ is identical to the number of modes $\phi_j^-$ . We can even choose the basis such that $\phi_j^- = \overline{\phi_j^+}$ and $\xi_j^- = - \xi_j^+$ for all $j\le N$ . In the following, we will always work with a basis $(\phi_1^+, ... , \phi_{N}^+$ , $\phi_1^-, ... , \phi_{N}^-)$ as described before and in (2.9).

We already noted that Property (a) of Definition 2.3 is generically satisfied. Property (b) demands that there is no nontrivial wave with vanishing flux. The existence of a wave with vanishing flux implies the existence of a nontrivial solution to the homogeneous radiation problem, which contradicts the uniqueness statement of Theorem 1.1. In this sense, Definition 2.3 (b) is a necessary condition for Theorem 1.1. The non-singularity of all frequencies $\omega$ is verified in certain settings. Theorem 5.3.2 of [Reference Nazarov and Plamenevsky19] provides also the orthogonality with respect to $Q^s$ . The orthogonality is derived also in [Reference Fliss and Joly9], see their Theorem 3.

Projections and radiation condition.

We proceed with the construction of function spaces and projections. For a non-singular frequency $\omega$ and basis functions as above, we define the following two subspaces of $H^1(W_0)$ ,

(2.10) \begin{equation} X_+ := \mathrm{span} \{ \phi_j^+ \,|\, 1\le j\le N \}\,,\quad X_- := \mathrm{span} \{ \phi_j^- \,|\, 1\le j\le N \}\,.\end{equation}

Every function $\phi^+\in X_+$ can be extended to a solution of the homogeneous problem. Here, some care should be taken, since a function in $X_+$ is, in general, not quasiperiodic for any $\xi$ . We construct as follows: Every basis function $\phi_j^+\in X_+$ has a $\xi_j^+$ -quasiperiodic extension. We denote the extension as $E_j^+ \phi_j^+$ , it is characterised by the property $E_j^+ \phi_j^+(x + m e_1) = e^{i m \xi_j^+} \phi_j^+(x)$ for every $m\in \mathbb{Z}$ . An arbitrary element $\phi^+\in X_+$ is a linear combination of basis elements, $\phi^+(x) := \sum_j \alpha_j \phi_j^+(x)$ for some coefficients $\alpha_j\in \mathbb{C},$ and we have to extend every basis function with the appropriate quasiperiodicity. More precisely, the extension of $\phi^+(x)$ as above is given by

\begin{equation*} (E \phi^+)(x) := \sum_j \alpha_j (E_j^+ \phi_j^+)(x)\,.\end{equation*}

This defines an extension operator E which maps elements of $X_+$ to solutions of the homogeneous problem $A \phi = \omega^2 \phi$ in $\Omega$ . Later on, we oftentimes simplify the notation and write again $\phi^+$ for the extension $E \phi^+$ . Analogously, extensions are defined for $\phi^-\in X_-$ .

Since the basis functions are linearly independent, there holds $X = X_+ \oplus X_-$ . An arbitrary element $u\in X$ can be written uniquely as $u = \sum_{j=1}^{N} \alpha_j \phi_j^+ + \sum_{j=1}^{N} \beta_j\phi_j^-$ . The natural projections $\Pi_{X,+} : X\to X_+ \subset X$ and $\Pi_{X,-} : X\to X_- \subset X$ are given by

\begin{equation*} \Pi_{X,+}(u) = \sum_{j=1}^{N} \alpha_j \phi_j^+\quad \text{ and }\quad \Pi_{X,-}(u) = \sum_{j=1}^{N} \beta_j \phi_j^-\,.\end{equation*}

We emphasise that the basis function $\phi_j^\pm$ is, in general, not $L^2$ -orthogonal. Accordingly, the projections are not necessarily $L^2$ -orthogonal projections.

The $L^2(W_0)$ -orthogonal projection onto the subspace X is denoted as $\Pi_X : L^2(W_0) \to L^2(W_0)$ . With the help of $\Pi_X,$ we define the two projections $\Pi_+ := \Pi_{X,+}\circ \Pi_X: L^2(W_0) \to L^2(W_0)$ onto $X_+$ and $\Pi_- := \Pi_{X,-}\circ \Pi_X: L^2(W_0) \to L^2(W_0)$ onto $X_-$ .

The case of two different periodic media.

Let us now discuss how the above concepts can be applied when a is given by $a^\mathrm{left}$ for $x_1< -R_0$ and by $a^\mathrm{right}$ for $x_1 > R_0$ . In this case, the spaces $X_\pm$ can be determined for $a^\mathrm{right}$ , which defines $X_\pm^\mathrm{right}$ , and for $a^\mathrm{left}$ , which defines $X_\pm^\mathrm{left}$ . Accordingly, we can define $\Pi_\pm^\mathrm{right}$ and $\Pi_\pm^\mathrm{left}$ , $Q^\mathrm{right}$ and $Q^\mathrm{left}$ , $\mathcal{Q}^\mathrm{right}$ and $\mathcal{Q}^\mathrm{left}$ . In order to take limits, it is still convenient to identify a function in $L^2(W_r)$ with a function in $L^2(W_0)$ . Nevertheless, one has to be careful in the definition of the forms Q, since we have no information on a in $W_0$ : The form $\mathcal{Q}^\mathrm{right}$ is defined as in (2.1), but with a replaced by $a^\mathrm{right}$ . Accordingly, on the left, $\mathcal{Q}^\mathrm{left}$ is defined as in (2.1) with the coefficient function $a^\mathrm{left}$ .

Radiation condition.

The projections allow to introduce the radiation condition that is used in this work. We remark that the equivalence with the usual radiation condition is established in Lemma 3.2. The norm $\| u \|_{sL}$ was introduced in (2.6).

Definition 2.4 (Radiation condition) Let $\omega$ be non-singular in the sense of Definition 2.3. For $r\in \mathbb{N}$ we consider boxes $W_{\pm r}$ and the corresponding projections $\Pi_\pm$ . We say that $u :\Omega \to \mathbb{C}$ with $\| u \|_{sL} < \infty$ satisfies the radiation condition if

(2.11) \begin{equation} \Pi_-(u|_{W_r}) \to 0\ \text{ and }\ \Pi_+(u|_{W_{-r}}) \to 0\ \text { as } r\to +\infty\,. \end{equation}

In this formula, we identify a function on $W_r$ with a function on $W_0$ via a shift. The convergence is that of $L^2(W_0)$ .

In the case of two different media at infinity, $a^\mathrm{right}$ and $a^\mathrm{left}$ , the condition (2.11) is modified in the natural way to

(2.12) \begin{equation} \Pi_-^\mathrm{right}(u|_{W_r}) \to 0\ \text{ and }\ \Pi_+^\mathrm{left}(u|_{W_{-r}}) \to 0\ \text { as } r\to +\infty\,. \end{equation}

2.3 Orthogonality

For notational convenience, we return to the discussion of one periodic medium a. The spaces $X_+$ and $X_-$ are not orthogonal in $L^2(W_0)$ . Nevertheless, we will obtain orthogonality with respect to the form $Q^s$ .

We have announced that the width $l\in \mathbb{N}$ of the boxes can be chosen arbitrarily. In this section, in order to derive the orthogonality, we will use l as a variable parameter. Here and below, we normalise the basis functions such that

(2.13) \begin{equation} \frac1{l} \int_{W_0} |\phi_j^\pm|^2 = 1\,.\end{equation}

A normalised basis function remains normalised when l is changed. This follows immediately from quasiperiodicity, which provides by its definition that $|\phi_j^\pm|^2$ is 1-periodic in $x_1$ .

Proposition 2.5 (Orthogonality). Every two different elements u and v of the set $\{ \phi_1^+, ... , \phi_{N}^+, \phi_1^-, ... , \phi_{N}^-\}$ satisfy

(2.14) \begin{equation} Q^s(u,v) = 0\,. \end{equation}

Proof. In the case that u and v have the same quasimoment $\xi$ , there holds $Q^s(u,v) = 0$ by the orthogonalisation of the basis functions. The construction was performed after Definition 2.3.

It remains to consider the case that u has the quasimoment $\xi$ and v has the quasimoment $\zeta\neq \xi$ . We want to calculate the expression

\begin{align*} Q^s(u, v) &= \frac1{2} \left( Q(u,v) - \overline{Q(v,u)} \right) = \frac1{2l} \int_{W_0} a\nabla u \cdot e_1 \bar v - \frac1{2l} \int_{W_0} a\nabla \bar v \cdot e_1 u\,. \end{align*}

Equation (2.4) of Lemma 2.1 shows that the sesquilinear form $Q^s$ is independent of the $x_1$ -position. This implies that $Q^s$ is independent of l.

With the notation $\Omega_{r_1, r_2} := (r_1, r_2) \times S,$ we calculate for the first expression

\begin{align*} &\frac1{2l} \int_{W_0} a\nabla u \cdot e_1 \bar v = \frac1{2l} \sum_{k=0}^{l-1} \int_{\Omega_{k,k+1}} a\nabla u \cdot e_1 \bar v\\ &\qquad = \frac1{2l} \sum_{k=0}^{l-1} \int_{\Omega_{0,1}} e^{ik\xi} a\nabla u\cdot e_1\, e^{-ik\zeta} \bar v = \frac1{2l} \sum_{k=0}^{l-1} e^{ik(\xi-\zeta)} \int_{\Omega_{0,1}} a\nabla u\cdot e_1\, \bar v\,. \end{align*}

The integral on the right is independent of l. With $\beta := e^{i(\xi-\zeta)}$ we write the factor in front of the integral as $\frac1{2l} \sum_{k=0}^{l-1} e^{ik(\xi-\zeta)} = \frac1{2l} \sum_{k=0}^{l-1} \beta^k = \frac1{2l} \frac{1-\beta^l}{1-\beta} \to 0$ for $\mathbb{N}\ni l\to \infty$ . Note that $\beta\neq 1$ is satisfied because of $\xi\neq \zeta$ . The other term is treated in the same way and we obtain (2.14).

Corollary 2.6 (Sign of the sesquilinear form). For some $\gamma>0$ holds

(2.15) \begin{equation} \pm \mathrm{Im}\, Q(u,u) \ge \frac{\gamma}{l} \| u \|_{L^2(W_0)}^2 \quad \forall\, u\in X_\pm\,. \end{equation}

Proof. Let $u\in X_+$ be arbitrary, $u = \sum_{j=1}^{N} \alpha_j \phi_j^+$ . We use $\gamma_+ := \min_j \mathrm{Im}\, \mathcal{Q}(\phi_j^+)$ , which is positive by (2.9). The orthogonality (2.14) allows to calculate

(2.16) \begin{equation} \mathrm{Im}\, Q(u,u) = \mathrm{Im}\, Q^s (u,u) = \sum_{j=1}^{N} |\alpha_j|^2\, \mathrm{Im}\, Q^s(\phi_j^+,\phi_j^+) \ge \gamma_+ \sum_{j=1}^{N} |\alpha_j|^2\,. \end{equation}

The immediate inequality $\| u \|_{L^2(W_0)}^2 \le C l \sum_{j=1}^{N} |\alpha_j|^2$ for a constant $C>0$ provides the claim in $X_+$ for $\gamma = \gamma_+/C > 0$ . The argument for $X_-$ is analogous.

We defined X to consist of restrictions of homogeneous solutions u on $\Omega$ . We now turn to a more quantitative version of this fact: If u is a homogeneous solution on a large subdomain, then its restriction is close to an element of X.

Lemma 2.7 (Outside a compact region, solutions are close to X). Let $l\in \mathbb{N}$ be fixed and let $\eta>0$ be an arbitrary error quantifier. There exists a large number $r_0 \in \mathbb{N}$ such that, for every $\mathbb{N}\ni r>r_0$ , there holds: Every function $u_r\in H^1_\mathrm{loc}(\Omega)$ with the properties

(2.17) \begin{equation} A u_r = \omega^2 u_r\text { in } \Omega_{-r,r}\quad \text{ and }\quad \| u_r \|_{sL} \le 1 \end{equation}

satisfies

(2.18) \begin{equation} \left\| u_r|_{W_0} - \Pi_X( u_r |_{W_0}) \right\|_{H^1(W_0)} \le \eta\,. \end{equation}

We will later use repeatedly the following immediate consequence of (2.18), which exploits $\Pi_X = \Pi_+ + \Pi_-$ :

(2.19) \begin{equation} \left\| u_r|_{W_0} - \Pi_+( u_r |_{W_0}) - \Pi_-( u_r |_{W_0}) \right\|_{L^2} \le \eta\,.\end{equation}

Proof. The aim is to show that $u_r|_{W_0}$ is near an element of X. We recall that l and $\eta$ are fixed. We want to show the existence of $r_0$ and argue by contradiction. If there is no $r_0$ with the desired property, then there exists a sequence $r\to \infty$ and a sequence of functions $u_r$ , which satisfy (2.17), but not (2.18). In the following, we work with this sequence and our aim is to derive a contradiction.

The boundedness of (2.17) allows to select a subsequence and to find a limit function u such that $u_r \to u$ converges weakly in $H^1(K)$ for every bounded subset of the form $K = (-l_0,l_0) \times S \subset \Omega$ , $l_0>0$ . From now on, we work with this subsequence. As a limit function, u also satisfies both properties of (2.17), the solution property and the boundedness. Locally, the sequence $u_r$ converges even strongly in $H^1$ , as can be shown easily by testing the equation for $u_r - u$ with $(u_r - u)\, \theta$ , where $\theta$ is a cut-off function. The strong convergence $u_r \to u$ in $H^1(W_0)$ implies that the limit u satisfies the same inequality as the approximate functions:

(2.20) \begin{equation} \left\| u|_{W_0} - \Pi_X( u |_{W_0}) \right\|_{H^1} \ge \eta\,. \end{equation}

This provides a contradiction: $u|_{W_0} \in X$ holds by definition of X in (2.7), so the left hand side of (2.20) vanishes.

We will later also exploit the $H^1$ -regularity of the elements $\phi\in X$ , where X is either $X^\mathrm{left}$ or $X^\mathrm{right}$ : For some constant C, there holds

(2.21) \begin{equation} \| \phi \|_{H^1(W_0)} \le C \| \phi \|_{L^2(W_0)}\end{equation}

for all elements $\phi\in X$ . The constant $C = C(\omega, \lambda)$ depends only on the frequency $\omega$ and on the ellipticity constant $\lambda$ of the coefficients. The property (2.21) can be obtained by testing the equation with the solution and a cut-off function, but it can be concluded for general C also immediately from the fact that the basis functions are of class $H^1(W_0)$ and that the space X is finite-dimensional.

3.1 An equivalent radiation condition

We next provide another formulation of the radiation condition. Indeed, in the literature, usually variants of (3.7) are used; one has some liberty in the choice of the precise convergence condition.

We describe the equivalence here in the setting of Theorem 1.1. Since the two directions $x_1 \to \pm \infty$ can be treated independently, the equivalence follows with the same proof also in the setting of Theorem 1.2.

Lemma 3.2 (Equivalent radiation condition). Let the coefficient a be as in Theorem 1.1, let $\omega>0$ be a non-singular frequency, let $u \in H^1_\mathrm{loc}(\Omega)$ be a function that satisfies (i) and (ii) of our solution concept, that is: u solves (1.1) in the sense of distributions and $\sup_{r\in \mathbb{Z}} \| u \|_{L^2((r,r+1)\times S)} < \infty$ .

The function u satisfies the radiation condition of Definition 2.4 if and only if the following holds: There exist $\phi_+\in X_+$ and $\phi_-\in X_-$ , which we identify with their extensions $E \phi_+$ and $E \phi_-$ , such that, as $r\to \infty$ ,

(3.7) \begin{equation} \| (u-\phi_+)|_{W_r} \|_{L^2(W_r)} \to 0\ \text{ and }\ \| (u-\phi_-)|_{W_{-r}} \|_{L^2(W_{-r})} \to 0\,. \end{equation}

Proof. The ‘if’-part. Let u satisfy (3.7) with $\phi_+\in X_+$ and $\phi_-\in X_-$ . Using a triangle inequality, boundedness of projections, and $\Pi_-(\phi_+|_{W_r}) = 0$ , we find

\begin{align*} \| \Pi_-(u|_{W_r}) \|_{L^2(W_r)} &\le \| \Pi_-((u-\phi_+)|_{W_r}) \|_{L^2(W_r)} + \| \Pi_-(\phi_+|_{W_r}) \|_{L^2(W_r)}\\[3pt] &\le C \| (u-\phi_+)|_{W_r} \|_{L^2(W_r)} \to 0 \end{align*}

by (3.7). This shows one part of (2.11) the calculation for $\Pi_+(u|_{W_{-r}})$ is analogous.

The ‘only-if’-part. Vice versa, let u satisfy the radiation condition (2.11). We consider the right boundary. For any sequence $R\to \infty$ , the sequences $u|_{W_R}$ are bounded in $L^2(W_0)$ by the assumption on the boundedness of the sL-norm. As a preparation of the proof, we subtract the right-going part: With the help of a projection, we define $\phi^R = \Pi_+(u|_{W_R})\in X_+$ (and we identify, as usual, $\phi^R$ with its extension as a solution on all of $\Omega$ , the extension operator is now the one that extends functions on $W_R$ ). We obtain $\Pi_+((u-\phi^R) |_{W_R}) = 0$ .

The sequence of functions $\phi^R |_{W_0}$ is bounded in $H^1(W_0)$ . We select a subsequence $R\to\infty$ (not relabelled) and a limit function $\phi_+$ with $\phi^R |_{W_0} \to \phi_+$ , weakly in $H^1(W_0)$ and strongly in $L^2(W_0)$ . The space $X_+$ is finite-dimensional and hence closed; we therefore have $\phi_+\in X_+$ . Once more, we identify $\phi_+$ with its extension $E \phi_+$ to a homogeneous solution on $\Omega$ . In particular, $\phi^R \to \phi_+$ holds locally on all of $\Omega$ . Our aim is to show, for an arbitrary sequence $r\to \infty$ , that $(u-\phi_+)|_{W_r} \to 0$ holds in $L^2$ . With that, (3.7) for the right half-axis is shown.

We fix an arbitrary error quantifier $\eta>0$ . A large number $r\in \mathbb{N}$ is chosen in dependence of $\eta$ , the choice is specified below.

We define $\phi^r$ corresponding to $u|_{W_r}$ as above, with $\Pi_+((u-\phi^r) |_{W_r}) = 0$ , and consider $w := w_r := u - \phi^r$ . We assume that the number r is sufficiently large such that the support of f is contained in $\{ x_1 < r\}$ . Then, w solves the homogeneous problem on $\Omega \cap \{ x_1 > r\}$ and hence satisfies the flux equality

(3.8) \begin{equation} \mathrm{Im}\, \mathcal{Q}(w|_{W_R}) = \mathrm{Im}\, \mathcal{Q}(w|_{W_r}) \end{equation}

for every number $R\in \mathbb{N}$ , $R>r+l$ .

Upper bound for the right hand side of (3.8). The difference $w|_{W_r} - \Pi_-(u|_{W_r}) = u|_{W_r} - \phi^r|_{W_r} - \Pi_-(u|_{W_r}) = u|_{W_r} - \Pi_X(u|_{W_r})$ is small by Lemma 2.7; more precisely, we achieve $\| w|_{W_r} - \Pi_-(u|_{W_r}) \|_{H^1} \le \eta$ when r is sufficiently large (large distance to the support of f). Together with the definition of $\mathcal{Q}$ , this allows to calculate the right hand side of (3.8) as

(3.9) \begin{align} \mathrm{Im}\, \mathcal{Q}(w|_{W_r}) &= \mathrm{Im}\, \mathcal{Q}(\Pi_-(u|_{W_r}) + [ w|_{W_r} - \Pi_-(u|_{W_r})] ) \nonumber\\[3pt] & \le \mathrm{Im}\, \mathcal{Q}(\Pi_-(u|_{W_r})) + C \eta \le C \eta\,. \end{align}

In this calculation, we inserted in a trivial way the function $\Pi_-(u|_{W_r})$ . We then used the definition of $\mathcal{Q}$ , in particular, its continuity on $H^1$ as a bilinear form, treating the squared bracket as an error term. In the last inequality we used $\mathrm{Im}\, \mathcal{Q}(\Pi_-(u|_{W_r})) \le 0$ of Corollary 2.6.

Lower bound for the left hand side of (3.8). We exploit that, for large R, the function $w|_{W_R}$ is close to an element of $X_+$ , which follows from the radiation condition. Let us make this fact precise: By definition of w, using $\Pi_+(\phi^r|_{W_R}) = \phi^r|_{W_R}$ , we find

\begin{align*} w|_{W_R} - \Pi_+(w|_{W_R}) &= u|_{W_R} - \phi^r|_{W_R} - \Pi_+(u|_{W_R}) + \Pi_+(\phi^r|_{W_R})\\[3pt] &= \left( u|_{W_R} - \Pi_X(u|_{W_R})\right) + \Pi_-(u|_{W_R}) \to 0 \end{align*}

as $R\to \infty$ . The smallness of the first bracket follows from Lemma 2.7 and the smallness of the last term from the radiation condition (2.11). The convergence is in $L^2$ , but the solution property allows once more to lift the regularity order and we obtain convergence also in $H^1$ . This can be used to calculate the left hand side of (3.8):

\begin{align*} \mathrm{Im}\, \mathcal{Q}(w|_{W_R}) &= \mathrm{Im}\, \mathcal{Q}(\Pi_+(w|_{W_R}) + [ w|_{W_R} - \Pi_+(w|_{W_R})] )\\[3pt] &\ge \mathrm{Im}\, \mathcal{Q}(\Pi_+(w|_{W_R})) + o(1) \ge \frac{\gamma}{l} \| \Pi_+(w|_{W_R}) \|_{L^2}^2 + o(1) \end{align*}

as $R\to \infty$ , where we used the quantitative estimate (2.15) in the last step.

Combining the calculations for the two sides of (3.8), we have obtained the smallness result

(3.10) \begin{equation} \| \Pi_+(w|_{W_R}) \|_{L^2}^2 \le \frac{Cl}{\gamma} \eta + o(1) \end{equation}

as $R\to \infty$ . We evaluate the left hand side:

\begin{equation*} \Pi_+(w|_{W_R}) = \Pi_+((u-\phi^r)|_{W_R}) = (\phi^R - \phi^r)|_{W_R}\,. \end{equation*}

The functions $\phi^R$ and $\phi^r$ are both extensions of elements in $X_+$ . This implies that also the difference $\phi^R - \phi^r$ is an extension of an element in $X_+$ , we may write it with the basis functions $\phi_j^+$ as $\phi^R - \phi^r = \sum_j \alpha_j \phi_j^+$ . For every $\rho$ , the norm of the restriction $(\phi^R - \phi^r)|_{W_\rho}$ is equivalent to the norm defined by $\left(\sum_{j\le N} |\alpha_j|^2\right)^{1/2}$ . In particular, $\| (\phi^R - \phi^r)|_{W_r} \|_{L^2}^2 \le C \| (\phi^R - \phi^r)|_{W_R}) \|_{L^2}^2$ for some constant C. Quasiperiodicity and relation (3.10) allow to calculate for the limit $R\to \infty$

\begin{align*} \| (\phi_+ - \phi^r)|_{W_r} \|_{L^2}^2 \leftarrow \| (\phi^R - \phi^r)|_{W_r} \|_{L^2}^2 &\le C \| (\phi^R - \phi^r)|_{W_R}) \|_{L^2}^2 \le \frac{Cl}{\gamma} \eta + o(1)\,. \end{align*}

It remains to exploit once more the radiation condition (2.11) and Lemma 2.7 to find $\| (u-\phi^r) |_{W_r}) \|_{L^2}^2 = \| u|_{W_r} - \Pi_+(u|_{W_r}) \|_{L^2}^2 \le \eta$ for sufficiently large r. Since we have shown that $\phi^r$ is close to $\phi_+$ , and since $\eta>0$ was arbitrary, we have shown the desired result $(u-\phi_+)|_{W_r} \to 0$ .

The condition on the left follows in the same way.

4.1 Conditional existence for the truncated problem

We now turn to existence properties. As in a Fredholm alternative, the uniqueness property can imply an existence result. We use a limiting absorption principle to derive this fact.

Proof. We use a limiting absorption principle. For every $\delta>0$ , we define a modified sesquilinear form by setting

(4.4) \begin{align} \beta_\delta(u,v) := &\int_{\Omega_{-L-l,R+l}} a\nabla u \nabla \bar v \vartheta - \int_{\Omega_{-L-l,R+l}} (\omega^2+i\delta)\, u \bar v \vartheta \nonumber\\[3pt] &\qquad- Q^\mathrm{right}(u|_{W_R}, v|_{W_R}) + Q^\mathrm{left}(u|_{W_{-L-l}}, v|_{W_{-L-l}})\,. \end{align}

Step 1: Solution for $\delta> 0$ . We claim that the sesquilinear form $\beta_\delta$ is coercive on $V_{L,R}$ . For $u\in V_{L,R,}$ we first calculate

\begin{align*} \mathrm{Im}\, \beta_\delta(u,u) &= \mathrm{Im}\, \int_{\Omega_{-L-l,R+l}} a\nabla u\cdot \nabla u \vartheta - \mathrm{Im}\, \int_{\Omega_{-L-l,R+l}} (\omega^2+i\delta)\, |u|^2 \vartheta \\[3pt] &\qquad- \mathrm{Im}\, \mathcal{Q}^\mathrm{right}(u|_{W_R}) + \mathrm{Im}\, \mathcal{Q}^\mathrm{left}(u|_{W_{-L-l}}) \\[3pt] &\le - \int_{\Omega_{-L-l,R+l}} \delta\, |u|^2 \vartheta - \frac{\gamma}{l} \| u|_{W_R} \|_{L^2}^2 - \frac{\gamma}{l} \| u|_{W_{-L-l}} \|_{L^2}^2 \,, \end{align*}

where we have used (2.15). This shows the coercivity inequality

(4.5) \begin{equation} -\mathrm{Im}\, \beta_\delta(u,u) \ge \gamma(\delta) \| u \|_{L^2(\Omega_{-L-l,R+l})}^2 \end{equation}

for $\gamma(\delta) := \min \{\delta, \gamma/l\} > 0$ . Let us now consider the real part of $\beta_\delta(u,u)$ . From (4.4) with $v= u$ we obtain, for a constant $C_0>0$ that depends only on $\lambda$ , $\Lambda$ and $\omega$ ,

(4.6) \begin{align} &\mathrm{Re}\, \beta_\delta(u,u) \ge \lambda \| \nabla u\|_{L^2(\Omega_{-L,R})}^2 - C_0 \left(\| u\|_{L^2(\Omega_{-L-l,R+l})}^2 + \| u|_{W_R} \|_{H^1}^2 + \| u|_{W_{-L-l}} \|_{H^1}^2\right)\nonumber\\[3pt] &\qquad \ge \lambda \| \nabla u\|_{L^2(\Omega_{-L,R})}^2 - C \| u\|_{L^2(\Omega_{-L-l,R+l})}^2 \,, \end{align}

where we used the definitions of $\mathcal{Q}^\mathrm{right}$ and $\mathcal{Q}^\mathrm{left}$ in the first inequality and the regularity property $\| \phi|_{W_0} \|_{H^1} \le C \| \phi|_{W_0} \|_{L^2}$ for $\phi\in X$ of (2.21) in the second inequality; for the latter we recall that, by definition of the space $V_{L,R}$ , the functions $u|_{W_R}$ and $u|_{W_{-L-l}}$ are in the spaces $X^\mathrm{left}$ and $X^\mathrm{right}$ .

We next calculate, using first (4.6) and $C_1 = C_1(R,L,C_0,\lambda)$ , then once more the regularity property of (2.21) and a corresponding constant $C_2 = C_2(C_1)$ , and finally (4.5):

\begin{align*} &\lambda \| u\|_{H^1(\Omega_{-L-l,R+l})}^2 \\[3pt] &\qquad \le C_1 \left( \mathrm{Re}\, \beta_\delta(u,u) + \| u\|_{L^2(\Omega_{-L-l,R+l})}^2 + \| u|_{W_R} \|_{H^1}^2 + \| u|_{W_{-L-l}} \|_{H^1}^2\right) \\[3pt] &\qquad \le C_2 \left( \mathrm{Re}\, \beta_\delta(u,u) + \| u\|_{L^2(\Omega_{-L-l,R+l})}^2 \right) \\[3pt] &\qquad \le C_2\, \mathrm{Re}\, \beta_\delta(u,u) - \frac{C_2}{\gamma(\delta)} \mathrm{Im}\, \beta_\delta(u,u)\\[3pt] &\qquad = \mathrm{Re}\, \left[ C_2 \left( 1 + i \gamma(\delta)^{-1} \right) \beta_\delta(u,u)\right]\,. \end{align*}

This inequality ensures coercivity of $\beta_\delta$ on $V_{L,R}$ . We can apply the Lax-Milgram lemma and obtain that the equation $\beta_\delta(u_\delta , .) = \langle f, . \rangle$ can be solved with $u_\delta\in V_{L,R}$ for every $\delta>0$ . The solution satisfies

(4.7) \begin{equation} \| u_\delta \|_{H^1(\Omega_{-L-l,R+l})} \le C(\delta) \| f \|_{H^{-1}(\Omega)}\,. \end{equation}

We note that this estimate is not helpful for the limit process $\delta\to 0$ since $C(\delta) \sim 1/\gamma(\delta)\to \infty$ for $\delta\to 0$ .

Step 2: Limit $\delta\to 0$ . In order to perform the limit, we distinguish two cases. The distinction regards the numbers

(4.8) \begin{equation} N_\delta := \| u_\delta \|_{L^2(W_{-L-l,R+l})}\,. \end{equation}

Case 1: $N_\delta$ bounded along a subsequence. If $N_\delta$ is bounded along a subsequence, then we choose this subsequence $\delta\to 0$ . The sequence $u_\delta$ is not only bounded in $L^2$ , but also in $H^1$ ; this can be concluded by taking the real part of $\beta_\delta(u_\delta, u_\delta) =\langle f, u_\delta \rangle$ , and using (2.21); we refer to the detailed argument in (4.6). We therefore find a limit function u and a further subsequence $\delta\to 0$ such that $u_\delta\rightharpoonup u$ weakly in $H^1(W_{-L-l,R+l})$ .

The properties $u|_{W_R} \in X_+^\mathrm{right}$ and $u|_{W_{-L-l}} \in X_-^\mathrm{left}$ are satisfied, since all $u_\delta$ satisfy these properties. This shows $u\in V_{L,R}$ . The weak convergence $u_\delta \rightharpoonup u$ is sufficient to take the limit $\delta\to 0$ in the relation $\beta_\delta(u_\delta, \varphi) = \langle f, \varphi \rangle$ , and we obtain $\beta(u, \varphi) = \langle f, \varphi \rangle$ . This shows that u is a solution of the truncated problem, and the existence statement is shown.

Case 2: $N_\delta\to \infty$ . In this case, we study the normalised functions $v_\delta := N_\delta^{-1} u_\delta$ . The sequence $v_\delta$ has all the properties of $u_\delta$ in the first case: The boundedness implies the existence of a limit function v (weak limit in $H^1$ and strong limit in $L^2$ ). Since $v_\delta$ solves the truncated problem with $f_\delta = N_\delta^{-1} f$ , the limit v solves $\beta(v, \varphi) =\langle 0, \varphi \rangle$ . Uniqueness for the truncated problem implies $v=0$ . We find a contradiction since $v_\delta$ has $L^2$ -norm 1 and converges strongly to $v=0$ . Case 2 cannot occur.

4.2 Radiation conditions for limits

We have constructed a truncated problem that can be solved with standard methods. The test whether or not the truncated problem was chosen appropriately lies in the question: Do limits of solutions to the truncated problem satisfy the radiation condition?

In the proof below, we use a flux equality which was, at least formally, not yet observed: Differences also satisfies a flux equality. We speak here of differences of two solutions, one to the truncated problem and one to the original problem. The proof is along the same lines as in the other flux equalities, and we therefore moved this elementary observation to the appendix, see Lemma A.1.

Proof. In this proof, we treat only the right boundary and the left boundary can be treated analogously. Correspondingly, we only use the notation Q and $\mathcal{Q}$ of the setting of Theorem 1.1. In the setting of Theorem 1.2,we should everywhere write $Q^\mathrm{right}$ and $\mathcal{Q}^\mathrm{right}$ .

We suppress the subscript k in the following and write R and L instead of $R_k$ and $L_k$ . As solutions to the truncated problems, the functions $u_k$ satisfy $u_k \in V_{L,R}$ , in particular $u_k\in H^1(\Omega_{-L-l,R+l})$ , and $\beta(u_k, v) = \langle f, v\rangle$ for every $v \in V_{L,R}$ . It is clear that the local limit u solves the Helmholtz equation with source term f. Our aim is to verify the radiation condition.

A crucial step will be to derive the following property. Let $(r_k)_k$ be a sequence in $\mathbb{N}$ such that $r_k\to \infty$ with $R_k - r_k \to \infty$ . We will suppress the subscript k also in the sequence $r_k$ and claim that there holds, in $L^2(W_r)$ ,

(4.9) \begin{equation} \Pi_-( u_k|_{W_{r}} ) \to 0\,. \end{equation}

Step 1: Verification of (4.9). We choose an error quantifier $\eta>0$ .

As in other proofs, we use $\phi(x) := \sum_j \alpha_j \phi_j^+(x)$ with $\Pi_+((u_k - \phi)|_{W_r}) = 0$ ( $\phi$ is the projection onto the right-going part). We subtract this function from $u_k$ and consider in the following $w_k := u_k - \phi$ . We use the flux equality of Lemma A.1 with the positions r and R; this is possible for large k since f has compact support and r has the property $r\to \infty$ . Together with the positivity of (2.15), we have

(4.10) \begin{equation} \mathrm{Im}\, \mathcal{Q}(w_k|_{W_{r}}) = \mathrm{Im}\, \mathcal{Q}(w_k|_{W_{R}}) \ge 0\,. \end{equation}

We used that both $u_k$ and $\phi$ (and hence w) are right-going waves in $W_R$ .

We now study $w_k|_{W_r}$ and the left hand side of (4.10). Because of $r\to \infty$ and $R - r \to \infty$ , the function $w_k$ is a solution of the homogeneous problem on a large domain with centre in r. This allows to use inequality (2.18) with the result that $\left\| w_k |_{W_r} - \Pi_+( w_k |_{W_r}) - \Pi_-( w_k |_{W_r}) \right\|_{H^1} \le \eta$ for all $k\ge k_0(\eta)$ . We observe that $\Pi_+(w_k |_{W_r}) = \Pi_+(u_k |_{W_r}) - \Pi_+(\phi|_{W_r}) = 0$ vanishes. We are therefore in the situation that $\left\| w_k |_{W_r} - \Pi_-( w_k |_{W_r}) \right\|_{H^1} \le \eta$ is small, $w_k |_{W_r}$ is close to a left-going wave.

After these preparations, we next obtain a further smallness condition. The subsequent calculation starts with the positivity of the quadratic form, obtained in (4.10). The equality is a trivial insertion of the projection of $w_k$ . The first inequality of the second line exploits the definition of $\mathcal{Q}$ as an integral and the $\eta$ -smallness of the error term; we assume here $\eta\le 1$ in order to absorb the quadratic term into the linear term. The estimate (2.15) for $\mathcal{Q}$ on $X_-$ is used in the last inequality.

\begin{align*} 0 &\le \mathrm{Im}\, \mathcal{Q}(w_k|_{W_r}) = \mathrm{Im}\, \mathcal{Q}(\Pi_-( w_k |_{W_r}) + [w_k |_{W_r} - \Pi_-( w_k |_{W_r})])\\[3pt] &\le \mathrm{Im}\, \mathcal{Q}(\Pi_-( w_k |_{W_r})) + \frac{C \Lambda}{l} \eta \le -\frac{\gamma}{l} \| \Pi_-( w_k |_{W_r}) \|_{L^2}^2 + \frac{C \Lambda}{l} \eta\,. \end{align*}

The constant depends, among others, on the bound for $u_k$ . The calculation provides the smallness

\begin{equation*} \| \Pi_-( u_k |_{W_r}) \|_{L^2}^2 = \| \Pi_-( w_k |_{W_r}) \|_{L^2}^2 \le\frac{C \Lambda}{\gamma} \eta\,. \end{equation*}

Since $\eta>0$ was arbitrary, this provides the claim of (4.9).

Step 2: The radiation condition for u. We fix a sequence $r_m \to \infty$ as $m\to\infty$ . We will verify the radiation condition along this sequence.

Given the sequence $(r_m)_m$ , we can choose a subsequence of indices $(k_m)_m$ with $k_m\to \infty$ as $m\to\infty$ , satisfying the following properties: (a) $L_k, R_k\to \infty$ and $R_k - r_k \to \infty$ along the subsequence $k = k_m$ . (b) $\| (u_k - u)|_{W_r} \|_{L^2(W_r)} \to 0$ as $m\to \infty$ along the sequences $k = k_m$ and $r= r_m$ . Property (b) can be satisfied because of the local convergence $u_k \to u$ : For fixed $r_m$ , we can choose $k = k_m$ such that the error is smaller than $1/m$ .

In the following, we fix the subsequence $(k_m)_m$ and omit the subscript m. The triangle inequality provides

\begin{align*} &\left\| \Pi_-( u|_{W_r} ) \right\|_{L^2(W_r)} \le \left\| \Pi_-( u_k|_{W_r} ) \right\|_{L^2(W_r)} + \left\| \Pi_-( u|_{W_r} ) - \Pi_-( u_k|_{W_r} ) \right\|_{L^2(W_r)}\,. \end{align*}

The first term vanishes by (4.9) as $k \to \infty$ . The second term is small by choice of the subsequence. This shows the smallness of the left hand side for large k and thus the radiation condition for u.

4.3 Limits of normalised solutions

We continue our investigation of limits of solutions to truncated problems. In the last section, we have seen that limits satisfy the radiation condition. In this section, we consider normalised solution sequences; our goal is to show that the limit of a normalised solution sequence is necessarily nontrivial. Technically, the lemma is used to show, with a contradiction argument, the uniqueness (and hence the existence) of solutions to truncated problems, see Corollary 4.7 below.

Lemma 4.6 (Limits of solutions to homogeneous truncated problems).

Let the setting be either that of Theorem 1.1 or that of Theorem 1.2. Let $u_k:\Omega\to \mathbb{C}$ be a normalised sequence of solutions to the truncated problems with $L_k, R_k$ and $f=0$ that converges locally:

(4.11) \begin{equation} \sup_{\rho} \| u_k |_{W_\rho} \|_{L^2(W_\rho)} = 1,\quad u_k\to u \quad \text{in} \quad H^1((-l_0,l_0)\times S) for \, every \, l_0 > 0 ,\end{equation}

the supremum is taken over all integers $\rho$ with $-L_k - l \le \rho\le R_k$ . Then, the limit u is a nontrivial radiating solution to $Au = \omega^2 u$ .

Proof. Because of the local convergence, there holds $\| u \|_{sL} \le 1$ . Since locally $u_k$ are solutions, also u is a distributional solution to $Au = \omega^2 u$ . Proposition 4.5 provides that u satisfies the radiation condition. The important information of Lemma 4.6 is $u\neq 0$ . We argue by contradiction and assume $u=0$ . We furthermore select a sequence $\rho = \rho(k)$ with $\| u_k |_{W_\rho} \|_{L^2(W_\rho)} = 1$ (the supremum is a maximum since $u_k$ is defined only on a bounded domain). We have to distinguish three cases.

Case 1: $\rho(k)$ bounded. If there exists a bounded subsequence $\rho(k)$ , then a further subsequence is constant: We find $\rho_0\in \mathbb{Z}$ such that $\rho(k) = \rho_0$ for all k along the new subsequence. Since $u_k\to u$ strongly in $L^2$ locally, the limit function u satisfies $\| u |_{W_{\rho_0}} \|_{L^2} = 1$ , and we find a contradiction to $u=0$ .

Case 2: $\rho(k)$ unbounded. Since Case 1 is excluded, we know $|\rho(k)|\to \infty$ . Without loss of generality, we assume that $\rho(k)\to \infty$ . Accordingly, in the following, Q and $\mathcal{Q}$ stand for $Q^\mathrm{right}$ and $\mathcal{Q}^\mathrm{right}$ .

To prepare the further arguments, we note that $u_k$ can be used as a test function for the truncated problem. Because of $f=0$ there holds $\beta(u_k, u_k) = \langle f, u_k\rangle = 0$ . Taking the imaginary part and exploiting the sign properties of $\mathcal{Q}$ yields $u_k|_{W_{R_k}} = u_k|_{W_{-L_k -l}} = 0$ .

Case 2a: Interior points. We assume that $R_k - \rho(k) \to \infty$ , which means that the critical point $\rho(k)$ has a large distance to both 0 and $R_k$ .

As in earlier proofs, we consider $\phi \in X_+$ , extended as a solution to all of $\Omega$ , with $\Pi_+((u_k-\phi)|_{W_{\rho}}) = 0$ . The difference $w_k := u_k - \phi$ satisfies the flux equality of Lemma A.1,

(4.12) \begin{equation} \mathrm{Im}\, \mathcal{Q}(w_k|_{W_\rho}) = \mathrm{Im}\, \mathcal{Q}(w_k|_{W_{R_k}}) \,. \end{equation}

The right hand side is positive because of $u_k|_{W_{R_k}}, \phi|_{W_{R_k}}\in X_+$ . Actually, $u_k|_{W_{R_k}}$ even vanishes (see the arguments in the beginning of Case 2); hence, only $\phi|_{W_{R_k}}$ remains in the argument. For the left hand side of (4.12), we use that, by choice of $\phi$ , there holds $\Pi_+(w_k|_{W_\rho}) = 0$ ; this implies the smallness of $w_k|_{W_\rho} - \Pi_-(w_k|_{W_\rho})$ by Lemma 2.7. The left hand side of (4.12) therefore can be calculated to satisfy $\mathrm{Im}\, \mathcal{Q}(w_k|_{W_\rho}) \le \mathrm{Im}\, \mathcal{Q}(\Pi_-(w_k|_{W_\rho})) + \eta$ for any small error quantifier $\eta>0$ . Equation (4.12) yields

\begin{align*} \mathrm{Im}\, \mathcal{Q}( \phi|_{W_{R_k}} ) - \mathrm{Im}\, \mathcal{Q}(\Pi_-(w_k|_{W_\rho})) \le \eta\,. \end{align*}

We obtain that both $\phi|_{W_{R_k}}$ (and hence $\Pi_+(u_k|_{W_{\rho}})$ ) and $\Pi_-(w_k|_{W_\rho}) = \Pi_-(u_k|_{W_\rho})$ are small. Using Lemma 2.7 again, we find a contradiction to $\| u_k |_{W_\rho} \|_{L^2(W_\rho)} = 1$ .

Case 2b: Large values close to boundaries. For a subsequence, the shifted sequence $\tilde u_k$ (shifted by $R_k$ ) consists of solutions to the homogeneous problem with vanishing Dirichlet data on $\{0\} \times S$ , but not vanishing in some subdomain, $\| \tilde u_k |_{W_{-D}} \|_{L^2(W_{-D})} = 1$ for all k and for some $D\in \mathbb{N}$ . We find a local limit function $\tilde u$ . The limit shares the above properties of $\tilde u_k$ .

For every $L_0$ , the solutions $\tilde u_k |_{W_{-R_k+L_0}}$ converge to 0 by assumption (local convergence of $u_k$ to $u=0$ ). The usual argument (subtracting the right-going part $\phi$ from $\tilde u_k$ ) we find that $\tilde u_k |_{W_{r_k}}$ converges to 0 for any sequence $r_k$ with $r_k \to \infty$ and $R_k -r_k\to \infty$ .

This implies that the limit $\tilde u$ vanishes as $x_1 \to -\infty$ , but is different from 0 on $W_{-D}$ . With an odd extension of $\tilde u$ , we see that this is in contradiction to (a) of Definition 2.3.

We mention that the above proof, in particular regarding the Cases 2a and 2b, has strong similarities with the proof of Lemma 5.1 and its Cases 2a and 2b, see below. Since the arguments are slightly more quantitative in the proof of Lemma 5.1, the reader might want to compare that proof for more details.

4.4 Uniqueness for truncated problems along a subsequence

This section is devoted to a uniqueness result for truncated problems. This is particularly useful since, by Lemma 4.4, uniqueness implies also existence of solutions. The following result improves Remark 4.3 in the direction that we do not have to choose $L_k$ and $R_k$ in an appropriate way to obtain uniqueness, but all sequences will guarantee uniqueness, at least for all sufficiently large indices k.

Proof. We argue by contradiction. The sequences $\mathbb{N}\ni R_k, L_k \to \infty$ are fixed, and we want to obtain the existence of $k_0$ . Assuming that no $k_0$ with the desired properties exists, there must exist a subsequence $k\to \infty$ such that the truncated problems for parameters $(L_{k}, R_{k})$ possess a nontrivial solution $u_k$ to $f=0$ . We normalise $u_k$ to have $\sup_{\rho} \| u_k |_{W_\rho} \|_{L^2(W_\rho)} = 1$ as in Lemma 4.6. We can extract a further subsequence $k\to \infty$ and a limit function u such that $u_k\to u$ locally in $H^1$ (at first, one concludes weak convergence in $H^1$ on every subset of the form $(-l_0,l_0)\times S\subset \Omega$ , then, by regularity of solutions, also strong convergence in $H^1$ on such sets). Lemma 4.6 provides that the limit function u is a nontrivial radiating solution to $Au = \omega^2 u$ .

In the situation of Theorem 1.1, Proposition 3.1 yields that the radiation problem on $\Omega$ for $f=0$ has only the trivial solution. This provides the desired contradiction. In the situation of Theorem 1.2, we have excluded the existence of such a function in the assumptions.

In both situations, we find the desired contradiction and conclude that there cannot exist sequences $L_k, R_k\to \infty$ with non-uniqueness.

The existence statement follows from Lemma 4.4.

Let us illustrate with an example that Corollary 4.7 improves the observation of Remark 4.3. We consider the elementary case of $A = - \Delta$ in dimension $d=1$ . Every $\omega>0$ is non-singular in the sense of Definition 2.3: The two basis functions are $\phi_1^\pm = e^{\pm i \omega x}$ and, with $m := \max \{n\in \mathbb{N}| 2\pi n\le \omega\}$ , the quasimoments are $\xi_1^+ = \omega - 2\pi m$ and $\xi_1^- = -\xi_1^+$ . We check that $\mathcal{Q}(\phi_1^+) = \frac1{l} \int_0^l \partial_x\phi_1^+\overline{\phi_1^+} = i\omega$ and $\mathcal{Q}(\phi_1^-) = - i\omega$ .

In the above setting, we study the linear combination $v(x) := \phi_1^+(x) + \phi_1^-(x) = 2 \cos(\omega x)$ . For $R=L \in (\pi/\omega) (\mathbb{N} + \frac12)$ , the function v solves the Dirichlet problem that was obtained in Remark 4.3. We see that resonances can occur even for large numbers R and L.

Our example makes clear that Corollary 4.7 is a surprising and strong result: Even if the values of R and L allow for some resonance phenomenon, the solution to the truncated problem is nevertheless unique. The point in the above construction is that v is a solution of a Dirichlet problem, but neither v nor any extension of it is a solution to the truncated domain problem.