A **Bloch wave** (also called **Bloch state** or **Bloch function** or **Bloch wave function**), named after Swiss physicist Felix Bloch, is a type of wavefunction for a particle in a periodically-repeating environment, most commonly an electron in a crystal. A wavefunction ψ is a Bloch wave if it has the form:

ψ
(
r
)
=
e
i
k
⋅
r
u
(
r
)
where **r** is position, ψ is the Bloch wave, *u* is a periodic function with the same periodicity as the crystal, **k** is a vector of real numbers called the crystal wave vector, *e* is Euler's number, and *i* is the imaginary unit. In other words, if you multiply a plane wave by a periodic function, you get a Bloch wave.

Bloch waves are important because of **Bloch's theorem**, which states that the energy eigenstates for an electron in a crystal can be written as Bloch waves. (More precisely, it states that the electron wave functions in a crystal have a basis consisting entirely of Bloch wave energy eigenstates.) This fact underlies the concept of electronic band structures.

These Bloch wave energy eigenstates are written with subscripts as ψ_{n k}, where *n* is a discrete index, called the *band index*, which is present because there are many different Bloch waves with the same **k** (each has a different periodic component *u*). Within a band (i.e., for fixed *n*), ψ_{n k} varies continuously with **k**, as does its energy. Also, for any reciprocal lattice vector **K**, ψ_{n k} = ψ_{n,(k+K)}. Therefore, all distinct Bloch waves occur for **k**-values within the first Brillouin zone of the reciprocal lattice.

The most common example of Bloch's theorem is describing electrons in a crystal. However, a Bloch-wave description applies more generally to any wave-like phenomenon in a periodic medium. For example, a periodic dielectric in electromagnetism leads to photonic crystals, and a periodic acoustic medium leads to phononic crystals. It is generally treated in the various forms of the dynamical theory of diffraction.

Suppose an electron is in a Bloch state

ψ
(
r
)
=
e
i
k
⋅
r
u
(
r
)
,

where *u* is periodic with the same periodicity as the crystal lattice. The actual quantum state of the electron is entirely determined by ψ, not **k** or *u* directly. This is important because **k** and *u* are *not* unique. Specifically, if ψ can be written as above using **k**, it can *also* be written using (**k** + **K**), where **K** is any reciprocal lattice vector (see figure at right). Therefore, wave vectors that differ by a reciprocal lattice vector are equivalent, in the sense that they characterize the same set of Bloch states.

The first Brillouin zone is a restricted set of **k**-vectors with the property that no two of them are equivalent, yet every possible **k** is equivalent to one (and only one) vector in the first Brillouin zone. Therefore, if we restrict **k** to the first Brillouin zone, then every Bloch state has a unique **k**. Therefore, the first Brillouin zone is often used to depict all of the Bloch states without redundancy, for example in a band structure, and it is used for the same reason in many calculations.

When **k** is multiplied by the reduced Planck's constant, it equals the electron's crystal momentum. Related to this, the group velocity of an electron can be calculated based on how the energy of a Bloch state varies with **k**; for more details see crystal momentum.

For a detailed example in which the consequences of Bloch's theorem are worked out in a specific situation, see the article: Particle in a one-dimensional lattice (periodic potential).

Next, we prove Bloch's theorem:

The defining property of a crystal is translational symmetry, which means that if the crystal is shifted an appropriate amount, it winds up with all its atoms in the same places. (A finite-size crystal cannot have perfect translational symmetry, but it is a useful approximation.)

A three-dimensional crystal has three *primitive lattice vectors* **a**_{1}, **a**_{2}, **a**_{3}. If the crystal is shifted by any of these three vectors, or a combination of them of the form

n
1
a
1
+
n
2
a
2
+
n
3
a
3

where *n*_{i} are three integers, then the atoms end up in the same set of locations as they started.

Another helpful ingredient in the proof is the *reciprocal lattice vectors*. These are three vectors **b**_{1}, **b**_{2}, **b**_{3} (with units of inverse length), with the property that **a**_{i} · **b**_{i} = 2π, but **a**_{i} · **b**_{j} = 0 when *i* ≠ *j*. (For the formula for **b**_{i}, see reciprocal lattice vector.)

Let
T
^
n
1
,
n
2
,
n
3
denote a translation operator that shifts every wave function by the amount *n*_{1}**a**_{1} + *n*_{2}**a**_{2} + *n*_{3}**a**_{3} (as above, *n*_{j} are integers). The following fact is helpful for the proof of Bloch's theorem:

**Proof:** Assume that we have a wavefunction *ψ* which is an eigenstate of all the translation operators. As a special case of this,

ψ
(
r
+
a
j
)
=
C
j
ψ
(
r
)
for *j* = 1, 2, 3, where *C*_{j} are three numbers (the eigenvalues) which do not depend on **r**. It is helpful to write the numbers *C*_{j} in a different form, by choosing three numbers *θ*_{1}, *θ*_{2}, *θ*_{3} with *e*^{2πiθj} = *C*_{j}:

ψ
(
r
+
a
j
)
=
e
2
π
i
θ
j
ψ
(
r
)
Again, the *θ*_{j} are three numbers which do not depend on **r**. Define **k** = *θ*_{1}**b**_{1} + *θ*_{2}**b**_{2} + *θ*_{3}**b**_{3}, where **b**_{j} are the reciprocal lattice vectors (see above). Finally, define

u
(
r
)
=
e
−
i
k
⋅
r
ψ
(
r
)
.
Then

u
(
r
+
a
j
)
=
e
−
i
k
⋅
(
r
+
a
j
)
ψ
(
r
+
a
j
)
=
(
e
−
i
k
⋅
r
e
−
i
k
⋅
a
j
)
(
e
2
π
i
θ
j
ψ
(
r
)
)
=
e
−
i
k
⋅
r
e
−
2
π
i
θ
j
e
2
π
i
θ
j
ψ
(
r
)
=
u
(
r
)
.

This proves that *u* has the periodicity of the lattice. Since *ψ*(**r**) = *e*^{i k · r}*u*(**r**), that proves that the state is a Bloch wave.

Finally, we are ready for the main proof of Bloch's theorem.

As above, let
T
^
n
1
,
n
2
,
n
3
denote a *translation operator* that shifts every wave function by the amount *n*_{1}**a**_{1} + *n*_{2}**a**_{2} + *n*_{3}**a**_{3}, where *n*_{i} are integers. Because the crystal has translational symmetry, this operator commutes with the Hamiltonian operator. Moreover, every such translation operator commutes with every other. Therefore, there is a simultaneous eigenbasis of the Hamiltonian operator and every possible
T
^
n
1
,
n
2
,
n
3
operator. This basis is what we are looking for. The wavefunctions in this basis are energy eigenstates (because they are eigenstates of the Hamiltonian), and they are also Bloch waves (because they are eigenstates of the translation operators; see Lemma above).

The concept of the Bloch state was developed by Felix Bloch in 1928, to describe the conduction of electrons in crystalline solids. The same underlying mathematics, however, was also discovered independently several times: by George William Hill (1877), Gaston Floquet (1883), and Alexander Lyapunov (1892). As a result, a variety of nomenclatures are common: applied to ordinary differential equations, it is called Floquet theory (or occasionally the *Lyapunov–Floquet theorem*). Various one-dimensional periodic potential equations have special names, for example, Hill's equation:

where the *θ*_{n} are constants. Hill's equation is very general, as the *θ*-related terms may be viewed as a Fourier series expansion of a periodic potential. Other much studied periodic one-dimensional equations are the Kronig–Penney model and Mathieu's equation.

Mathematically Bloch's theorem is interpreted in terms of unitary characters of a lattice group, and is applied to spectral geometry.