Bessel functions, first defined by the mathematician Daniel Bernoulli and then generalized by Friedrich Bessel, are the canonical solutions y(x) of Bessel's differential equation

x^2 \frac{d^2 y}{dx^2} + x \frac{dy}{dx} + (x^2  \alpha^2)y = 0
for an arbitrary complex number α (the order of the Bessel function). Although α and −α produce the same differential equation for real α, it is conventional to define different Bessel functions for these two values in such a way that the Bessel functions are mostly smooth functions of α.
The most important cases are for α an integer or halfinteger. Bessel functions for integer α are also known as cylinder functions or the cylindrical harmonics because they appear in the solution to Laplace's equation in cylindrical coordinates. Spherical Bessel functions with halfinteger α are obtained when the Helmholtz equation is solved in spherical coordinates.
Contents

Applications of Bessel functions 1

Definitions 2

Bessel functions of the first kind: Jα 2.1

Bessel's integrals 2.1.1

Relation to hypergeometric series 2.1.2

Relation to Laguerre polynomials 2.1.3

Bessel functions of the second kind: Yα 2.2

Hankel functions: Hα(1), Hα(2) 2.3

Modified Bessel functions: Iα, Kα 2.4

Spherical Bessel functions: jn, yn 2.5

Generating function 2.5.1

Differential relations 2.5.2

Spherical Hankel functions: hn(1), hn(2) 2.6

Riccati–Bessel functions: Sn, Cn, ξn, ζn 2.7

Asymptotic forms 3

Properties 4

Multiplication theorem 5

Bourget's hypothesis 6

Selected identities 7

See also 8

Notes 9

References 10

External links 11
Applications of Bessel functions
Bessel's equation arises when finding separable solutions to Laplace's equation and the Helmholtz equation in cylindrical or spherical coordinates. Bessel functions are therefore especially important for many problems of wave propagation and static potentials. In solving problems in cylindrical coordinate systems, one obtains Bessel functions of integer order (α = n); in spherical problems, one obtains halfinteger orders (α = n+1/2). For example:
Bessel functions also appear in other problems, such as signal processing (e.g., see FM synthesis, Kaiser window, or Bessel filter).
Definitions
Because this is a secondorder differential equation, there must be two linearly independent solutions. Depending upon the circumstances, however, various formulations of these solutions are convenient. Different variations are summarized in the table below, and described in the following sections.
Type

First kind

Second kind

Bessel functions

_{α}J

_{α}Y

modified Bessel functions

I_{α}

K_{α}

Hankel functions

H_{α}^{(1)} = J_{α} + iY_{α}

H_{α}^{(2)} = J_{α}  iY_{α}

Spherical Bessel functions

j_{n}

y_{n}

Spherical Hankel functions

h_{n}^{(1)} = j_{n} + iy_{n}

h_{n}^{(2)} = j_{n}  iy_{n}

Bessel functions of the first kind: J_{α}
Bessel functions of the first kind, denoted as J_{α}(x), are solutions of Bessel's differential equation that are finite at the origin (x = 0) for integer or positive α, and diverge as x approaches zero for negative noninteger α. It is possible to define the function by its series expansion around x = 0, which can be found by applying the Frobenius method to Bessel's equation:^{[1]}

J_\alpha(x) = \sum_{m=0}^\infty \frac{(1)^m}{m! \, \Gamma(m+\alpha+1)} {\left(\frac{x}{2}\right)}^{2m+\alpha}
where Γ(z) is the gamma function, a shifted generalization of the factorial function to noninteger values. The Bessel function of the first kind is an entire function if α is an integer, otherwise it is a multivalued function with singularity at zero. The graphs of Bessel functions look roughly like oscillating sine or cosine functions that decay proportionally to 1/√x (see also their asymptotic forms below), although their roots are not generally periodic, except asymptotically for large x. (The series indicates that −J_{1}(x) is the derivative of J_{0}(x), much like −sin(x) is the derivative of cos(x); more generally, the derivative of J_{n}(x) can be expressed in terms of J_{n±1}(x) by the identities below.)
Plot of Bessel function of the first kind, J_{α}(x), for integer orders α = 0, 1, 2
For noninteger α, the functions J_{α}(x) and J_{−α}(x) are linearly independent, and are therefore the two solutions of the differential equation. On the other hand, for integer order α, the following relationship is valid (note that the Gamma function has simple poles at each of the nonpositive integers):^{[2]}

J_{n}(x) = (1)^n J_{n}(x).\,
This means that the two solutions are no longer linearly independent. In this case, the second linearly independent solution is then found to be the Bessel function of the second kind, as discussed below.
Bessel's integrals
Another definition of the Bessel function, for integer values of n, is possible using an integral representation:^{[3]}

J_n(x) = \frac{1}{\pi} \int_0^\pi \cos (n \tau  x \sin(\tau)) \,d\tau.
Another integral representation is:^{[3]}

J_n (x) = \frac{1}{2 \pi} \int_{\pi}^\pi e^{i(n \tau  x \sin(\tau))} \,d\tau.
This was the approach that Bessel used, and from this definition he derived several properties of the function. The definition may be extended to noninteger orders by (for Re(x) > 0), one of Schläfli's integrals:^{[3]}

J_\alpha(x) = \frac{1}{\pi} \int_0^\pi \cos(\alpha\tau x \sin\tau)\,d\tau  \frac{\sin(\alpha\pi)}{\pi} \int_0^\infty e^{x \sinh(t)  \alpha t} \, dt. ^{[4]}^{[5]}^{[6]}^{[7]}
Relation to hypergeometric series
The Bessel functions can be expressed in terms of the generalized hypergeometric series as^{[8]}

J_\alpha(x)=\frac{(\frac{x}{2})^\alpha}{\Gamma(\alpha+1)} \;_0F_1 (\alpha+1; \tfrac{x^2}{4}).
This expression is related to the development of Bessel functions in terms of the Bessel–Clifford function.
Relation to Laguerre polynomials
In terms of the Laguerre polynomials L_{k} and arbitrarily chosen parameter t, the Bessel function can be expressed as^{[9]}

\frac{J_\alpha(x)}{\left( \frac{x}{2}\right)^\alpha}= \frac{e^{t}}{\Gamma(\alpha+1)} \sum_{k=0}^\infty \frac{L_k^{(\alpha)}\left( \frac{x^2}{4 t}\right)} \frac{t^k}{k!}.
Bessel functions of the second kind: Y_{α}
The Bessel functions of the second kind, denoted by Y_{α}(x), occasionally denoted instead by N_{α}(x), are solutions of the Bessel differential equation that have a singularity at the origin (x = 0) and are multivalued. These are sometimes called Weber functions as they were introduced by H. Weber (1873), and also Neumann functions after Carl Neumann.^{[10]}
Plot of Bessel function of the second kind, Y_{α}(x), for integer orders α = 0, 1, 2.
For noninteger α, Y_{α}(x) is related to J_{α}(x) by:

Y_\alpha(x) = \frac{J_\alpha(x) \cos(\alpha\pi)  J_{\alpha}(x)}{\sin(\alpha\pi)}.
In the case of integer order n, the function is defined by taking the limit as a noninteger α tends to n:

Y_n(x) = \lim_{\alpha \to n} Y_\alpha(x).
There is also a corresponding integral formula (for Re(x) > 0),^{[11]}

Y_n(x) =\frac{1}{\pi} \int_0^\pi \sin(x \sin\theta  n\theta) \, d\theta  \frac{1}{\pi} \int_0^\infty \left[ e^{n t} + (1)^n e^{n t} \right] e^{x \sinh t} \, dt.
Y_{α}(x) is necessary as the second linearly independent solution of the Bessel's equation when α is an integer. But Y_{α}(x) has more meaning than that. It can be considered as a 'natural' partner of J_{α}(x). See also the subsection on Hankel functions below.
When α is an integer, moreover, as was similarly the case for the functions of the first kind, the following relationship is valid:

Y_{n}(x) = (1)^n Y_n(x).\,
Both J_{α}(x) and Y_{α}(x) are holomorphic functions of x on the complex plane cut along the negative real axis. When α is an integer, the Bessel functions J are entire functions of x. If x is held fixed at a nonzero value, then the Bessel functions are entire functions of α.
The Bessel functions of the second kind when α is an integer is an example of the second kind of solution in Fuchs's theorem.
Hankel functions: H_{α}^{(1)}, H_{α}^{(2)}
Another important formulation of the two linearly independent solutions to Bessel's equation are the Hankel functions of the first and second kind, H_{α}^{(1)}(x) and H_{α}^{(2)}(x), defined by:^{[12]}

H_\alpha^{(1)}(x) = J_\alpha(x)+iY_\alpha(x)

H_\alpha^{(2)}(x) = J_\alpha(x)iY_\alpha(x)
where i is the imaginary unit. These linear combinations are also known as Bessel functions of the third kind; they are two linearly independent solutions of Bessel's differential equation. They are named after Hermann Hankel.
The importance of Hankel functions of the first and second kind lies more in theoretical development rather than in application. These forms of linear combination satisfy numerous simplelooking properties, like asymptotic formulae or integral representations. Here, 'simple' means an appearance of the factor of the form e^{if(x)}. The Bessel function of the second kind then can be thought to naturally appear as the imaginary part of the Hankel functions.
The Hankel functions are used to express outward and inwardpropagating cylindrical wave solutions of the cylindrical wave equation, respectively (or vice versa, depending on the sign convention for the frequency).
Using the previous relationships they can be expressed as:

H_\alpha^{(1)} (x) = \frac{J_{\alpha} (x)  e^{\alpha \pi i} J_\alpha (x)}{i \sin (\alpha \pi)}

H_\alpha^{(2)} (x) = \frac{J_{\alpha} (x)  e^{\alpha \pi i} J_\alpha (x)}{ i \sin (\alpha \pi)}.
If α is an integer, the limit has to be calculated. The following relationships are valid, whether α is an integer or not:^{[13]}

H_{\alpha}^{(1)} (x)= e^{\alpha \pi i} H_\alpha^{(1)} (x)

H_{\alpha}^{(2)} (x)= e^{\alpha \pi i} H_\alpha^{(2)} (x).
In particular, if α = m + 1/2 with m a nonnegative integer, the above relations imply directly that

J_{(m+\frac{1}{2})}(x) = (1)^{m+1} Y_{m+\frac{1}{2}}(x)

Y_{(m+\frac{1}{2})}(x) = (1)^m J_{m+\frac{1}{2}}(x).
These are useful in developing the spherical Bessel functions (below).
The Hankel functions admit the following integral representations for Re(x) > 0:^{[14]}

H_\alpha^{(1)} (x)= \frac{1}{\pi i}\int_{\infty}^{+\infty+i\pi} e^{x\sinh t  \alpha t} \, dt,

H_\alpha^{(2)} (x)= \frac{1}{\pi i}\int_{\infty}^{+\inftyi\pi} e^{x\sinh t  \alpha t} \, dt,
where the integration limits indicate integration along a contour that can be chosen as follows: from −∞ to 0 along the negative real axis, from 0 to ±iπ along the imaginary axis, and from ±iπ to +∞±iπ along a contour parallel to the real axis.^{[15]}
Modified Bessel functions: I_{α}, K_{α}
The Bessel functions are valid even for complex arguments x, and an important special case is that of a purely imaginary argument. In this case, the solutions to the Bessel equation are called the modified Bessel functions (or occasionally the hyperbolic Bessel functions) of the first and second kind, and are defined by:^{[16]}

I_\alpha(x) = i^{\alpha} J_\alpha(ix) =\sum_{m=0}^\infty \frac{1}{m!\, \Gamma(m+\alpha+1)}\left(\frac{x}{2}\right)^{2m+\alpha}

K_\alpha(x) = \frac{\pi}{2} \frac{I_{\alpha} (x)  I_\alpha (x)}{\sin (\alpha \pi)},
when α is not an integer; when α is an integer, then the limit is used. These are chosen to be realvalued for real and positive arguments x. The series expansion for I_{α}(x) is thus similar to that for J_{α}(x), but without the alternating (−1)^{m} factor.
If −π < arg(x) ≤ π/2, K_{α}(x) can be expressed as a Hankel function of the first kind:

K_\alpha(x) = \frac{\pi}{2} i^{\alpha+1} H_\alpha^{(1)}(ix),
and if π/2 < arg(x) ≤ π, it can be expressed as a Hankel function of the second kind:

K_\alpha(x) = \frac{\pi}{2} (i)^{\alpha+1} H_\alpha^{(2)}(ix).
We can express the first and second Bessel functions in terms of the modified Bessel functions (these are valid if −π < arg(z) ≤ π/2):

\begin{align} J_\alpha(iz) &=e^{\frac{\alpha i\pi}{2}} I_\alpha(z)\\ Y_\alpha(iz) &=e^{\frac{(\alpha+1)i\pi}{2}}I_\alpha(z)\frac{2}{\pi}e^{\frac{\alpha i\pi}{2}}K_\alpha(z). \end{align}
I_{α}(x) and K_{α}(x) are the two linearly independent solutions to the modified Bessel's equation:^{[17]}

x^2 \frac{d^2 y}{dx^2} + x \frac{dy}{dx}  (x^2 + \alpha^2)y = 0.
Unlike the ordinary Bessel functions, which are oscillating as functions of a real argument, I_{α} and K_{α} are exponentially growing and decaying functions, respectively. Like the ordinary Bessel function J_{α}, the function I_{α} goes to zero at x = 0 for α > 0 and is finite at x = 0 for α = 0. Analogously, K_{α} diverges at x = 0 with the singularity being of logarithmic type.^{[18]}
Modified Bessel functions of 1st kind, I_{α}(x), for α = 0, 1, 2, 3

Modified Bessel functions of 2nd kind, K_{α}(x), for α = 0, 1, 2, 3

Two integral formulas for the modified Bessel functions are (for Re(x) > 0):^{[19]}

I_\alpha(x) = \frac{1}{\pi}\int_0^\pi \exp(x\cos(\theta)) \cos(\alpha\theta) \,d\theta  \frac{\sin(\alpha\pi)}{\pi}\int_0^\infty \exp(x\cosh t  \alpha t) \,dt ,

K_\alpha(x) = \int_0^\infty \exp(x\cosh t) \cosh(\alpha t) \,dt.
Modified Bessel functions K_{1/3} and K_{2/3} can be represented in terms of rapidly converged integrals^{[20]}

\begin{align} K_{\frac{1}{3}} (\xi) &= \sqrt{3}\, \int_0^\infty \, \exp \left[ \xi \left(1+\frac{4x^2}{3}\right) \sqrt{1+\frac{x^2}{3}} \,\right] \,dx \\ K_{\frac{2}{3}} (\xi) &= \frac{1}{ \sqrt{3}} \, \int_0^\infty \, \frac{3+2x^2}{\sqrt{1+\frac{x^2}{3}}} \exp \left[ \xi \left(1+\frac{4x^2}{3}\right) \sqrt{1+\frac{x^2}{3}} \,\right] \,dx.\end{align}
The modified Bessel function of the second kind has also been called by the nowrare names:
Spherical Bessel functions: j_{n}, y_{n}
Spherical Bessel functions of 1st kind, j_{n}(x), for n = 0, 1, 2
Spherical Bessel functions of 2nd kind, y_{n}(x), for n = 0, 1, 2
When solving the Helmholtz equation in spherical coordinates by separation of variables, the radial equation has the form:

x^2 \frac{d^2 y}{dx^2} + 2x \frac{dy}{dx} + [x^2  n(n+1)]y = 0.
The two linearly independent solutions to this equation are called the spherical Bessel functions j_{n} and y_{n}, and are related to the ordinary Bessel functions J_{n} and Y_{n} by:^{[22]}

j_{n}(x) = \sqrt{\frac{\pi}{2x}} J_{n+\frac{1}{2}}(x),

y_{n}(x) = \sqrt{\frac{\pi}{2x}} Y_{n+\frac{1}{2}}(x) = (1)^{n+1} \sqrt{\frac{\pi}{2x}} J_{n\frac{1}{2}}(x).
y_{n} is also denoted n_{n} or η_{n}; some authors call these functions the spherical Neumann functions.
The spherical Bessel functions can also be written as (Rayleigh's formulas):^{[23]}

j_n(x) = (x)^n \left(\frac{1}{x}\frac{d}{dx}\right)^n\,\frac{\sin(x)}{x} ,

y_n(x) = (x)^n \left(\frac{1}{x}\frac{d}{dx}\right)^n\,\frac{\cos(x)}{x}.
The first spherical Bessel function j_{0}(x) is also known as the (unnormalized) sinc function. The first few spherical Bessel functions are:

j_0(x)=\frac{\sin(x)} {x}

j_1(x)=\frac{\sin(x)} {x^2} \frac{\cos(x)} {x}

j_2(x)=\left(\frac{3} {x^2}  1 \right)\frac{\sin(x)}{x}  \frac{3\cos(x)} {x^2}^{[24]}

j_3(x)=\left(\frac{15}{x^3}  \frac{6}{x} \right)\frac{\sin(x)}{x} \left(\frac{15}{x^2}  1\right) \frac{\cos(x)} {x},
and

y_0(x)=j_{1}(x)=\,\frac{\cos(x)} {x}

y_1(x)=j_{2}(x)=\,\frac{\cos(x)} {x^2} \frac{\sin(x)} {x}

y_2(x)=j_{3}(x)=\left(\,\frac{3}{x^2}+1 \right)\frac{\cos(x)}{x} \frac{3\sin(x)} {x^2}^{[25]}

y_{3}\left( x\right)=j_{4}(x) =\left( \frac{15}{x^{3}}+\frac{6}{x}\right) \frac{\cos(x)}{x}\left( \frac{15}{x^{2}}1\right) \frac{\sin(x)}{x}.
Generating function
The spherical Bessel functions have the generating functions ^{[26]}

\frac 1 {z} \cos \left (\sqrt{z^2  2zt} \right )= \sum_{n=0}^\infty \frac{t^n}{n!} j_{n1}(z),

\frac 1 {z} \sin \left ( \sqrt{z^2 + 2zt} \right )= \sum_{n=0}^\infty \frac{(t)^n}{n!} y_{n1}(z) .
Differential relations
In the following f_{n} is any of j_n, y_n, h_n^{(1)}, h_n^{(2)} for n=0,\pm 1,\pm 2,\dots^{[27]}

\left(\frac{1}{z}\frac{d}{dz}\right)^m\left(z^{n+1}f_n(z)\right)=z^{nm+1}f_{nm}(z),

\left(\frac{1}{z}\frac{d}{dz}\right)^m\left(z^{n}f_n(z)\right)=(1)^m z^{nm}f_{n+m}(z).
Spherical Hankel functions: h_{n}^{(1)}, h_{n}^{(2)}
There are also spherical analogues of the Hankel functions:

h_n^{(1)}(x) = j_n(x) + i y_n(x) \,

h_n^{(2)}(x) = j_n(x)  i y_n(x). \,
In fact, there are simple closedform expressions for the Bessel functions of halfinteger order in terms of the standard trigonometric functions, and therefore for the spherical Bessel functions. In particular, for nonnegative integers n:

h_n^{(1)}(x) = (i)^{n+1} \frac{e^{ix}}{x} \sum_{m=0}^n \frac{i^m}{m!(2x)^m} \frac{(n+m)!}{(nm)!}
and h_n^{(2)} is the complexconjugate of this (for real x). It follows, for example, that j_0(x) = \sin(x)/x and y_0(x) = \cos(x)/x, and so on.
The spherical Hankel functions appear in problems involving spherical wave propagation, for example in the multipole expansion of the electromagnetic field.
Riccati–Bessel functions: S_{n}, C_{n}, ξ_{n}, ζ_{n}
Riccati–Bessel functions only slightly differ from spherical Bessel functions:

S_n(x)=x j_n(x)=\sqrt{\frac{\pi x}{2}} \, J_{n+\frac{1}{2}}(x)

C_n(x)=x y_n(x)=\sqrt{\frac{\pi x}{2}} \, Y_{n+\frac{1}{2}}(x)

\xi_n(x) = x h_n^{(1)}(x)=\sqrt{\frac{\pi x}{2}} \, H_{n+\frac{1}{2}}^{(1)}(x)=S_n(x)iC_n(x)

\zeta_n(x)=x h_n^{(2)}(x)=\sqrt{\frac{\pi x}{2}} \, H_{n+\frac{1}{2}}^{(2)}(x)=S_n(x)+iC_n(x).
They satisfy the differential equation:

x^2 \frac{d^2 y}{dx^2} + [x^2  n (n+1)] y = 0.
For example, this kind of differential equation appears in Quantum Mechanics while solving the radial component of the Schrodinger's Equation with hypothetical cylindrical infinite potential barrier. For reference see p. 154, Introduction to Quantum Mechanics by Griffiths, 2nd Edition. This differential equation, and the Riccati–Bessel solutions, also arises in the problem of scattering of electromagnetic waves by a sphere, known as Mie scattering after the first published solution by Mie (1908). See e.g., Du (2004)^{[28]} for recent developments and references.
Following Debye (1909), the notation \psi_n,\chi_n is sometimes used instead of S_n,C_n.
Asymptotic forms
The Bessel functions have the following asymptotic forms. For small arguments^{[1]} 0 < z \ll \sqrt{\alpha + 1}, one obtains, when α is not a negative integer:

J_\alpha(z) \sim \frac{1}{\Gamma(\alpha+1)} \left( \frac{z}{2} \right) ^\alpha
When α is a negative integer, we have:

J_\alpha(z) \sim \frac{(1)^{\alpha}}{(\alpha)!} \left( \frac{2}{z} \right) ^\alpha
For the Bessel function of the second kind we have three cases:

Y_\alpha(z) \sim \begin{cases} \frac{2}{\pi} \left ( \ln \left (\frac{z}{2} \right ) + \gamma \right ) & \text{if } \alpha=0 \\ \\ \frac{\Gamma(\alpha)}{\pi} \left( \frac{2}{z} \right) ^\alpha+\frac{1}{\Gamma(\alpha+1)} \left( \frac{z}{2} \right) ^\alpha \cot(\alpha \pi) & \text{if } \alpha\text{ is not a nonpositive integer (one term dominates unless }\alpha\text{ is imaginary)}\\ \\ \frac{(1)^\alpha\Gamma(\alpha)}{\pi} \left( \frac{z}{2} \right) ^\alpha & \text{if } \alpha\text{ is a negative integer} \end{cases}
where γ is the Euler–Mascheroni constant (0.5772...).
For large real arguments x \gg \left \alpha^2  \tfrac{1}{4} \right , one cannot write a true asymptotic form for Bessel functions of the first and second kind (unless α is halfinteger) because they have zeros all the way out to infinity which would have to be matched exactly by any asymptotic expansion. However, for a given value of arg(z) one can write an equation containing a term of order z^{−1}:^{[29]}

\begin{align} J_\alpha(z) &= \sqrt{\frac{2}{\pi z}}\left(\cos \left(z\frac{\alpha\pi}{2}\frac{\pi}{4}\right)+e^{\operatorname{Im}(z)}O(z^{1})\right) && \text{ for } \arg z< \pi \\ Y_\alpha(z) &= \sqrt{\frac{2}{\pi z}}\left(\sin \left(z\frac{\alpha\pi}{2}\frac{\pi}{4}\right)+e^{\operatorname{Im}(z)}O(z^{1})\right) && \text{ for } \arg z< \pi. \end{align}
(For α = 1/2 the last terms in these formulas drop out completely; see the spherical Bessel functions above.) Even though these equations are true, better approximations may be available for complex z. For example, J_{0}(z) when z is near the negative real line is approximated better by

J_0(z)\approx\sqrt{\frac{2}{\pi z}}\cos \left(z+\frac{\pi}{4}\right)
than by

J_0(z)\approx\sqrt{\frac{2}{\pi z}}\cos \left(z\frac{\pi}{4}\right).
The asymptotic forms for the Hankel functions are:

\begin{align} H_\alpha^{(1)}(z) &\sim \sqrt{\frac{2}{\pi z}}\exp\left(i\left(z\frac{\alpha\pi}{2}\frac{\pi}{4}\right)\right) &&\text{ for } \pi<\arg z<2\pi \\ H_\alpha^{(2)}(z) &\sim \sqrt{\frac{2}{\pi z}}\exp\left(i\left(z\frac{\alpha\pi}{2}\frac{\pi}{4}\right)\right) && \text{ for } 2\pi<\arg z<\pi \end{align}
These can be extended to other values of arg(z) using equations relating H_\alpha^{(1)}(ze^{im\pi}) and H_\alpha^{(2)}(ze^{im\pi}) to H_{α}^{(1)}(z) and H_{α}^{(2)}(z).^{[30]} It is interesting that although the Bessel function of the first kind is the average of the two Hankel functions, J_{α}(z) is not asymptotic to the average of these two asymptotic forms when z is negative (because one or the other will not be correct there, depending on the arg(z) used). But the asymptotic forms for the Hankel functions permit us to write asymptotic forms for the Bessel functions of first and second kinds for complex (nonreal) z so long as z goes to infinity at a constant phase angle arg z (using the square root having positive real part):

\begin{align} J_\alpha(z) &\sim \frac{1}{\sqrt{2\pi z}} \exp\left( i\left(z\frac{\alpha\pi}{2}\frac{\pi}{4}\right)\right) && \text{ for } \pi < \arg z < 0 \\ J_\alpha(z) &\sim \frac{1}{\sqrt{2\pi z}} \exp\left(i\left(z\frac{\alpha\pi}{2}\frac{\pi}{4}\right)\right) && \text{ for } 0 < \arg z < \pi \\ Y_\alpha(z) &\sim i\frac{1}{\sqrt{2\pi z}} \exp\left( i\left(z\frac{\alpha\pi}{2}\frac{\pi}{4}\right)\right) && \text{ for } \pi < \arg z < 0 \\ Y_\alpha(z) &\sim i\frac{1}{\sqrt{2\pi z}} \exp\left(i\left(z\frac{\alpha\pi}{2}\frac{\pi}{4}\right)\right) && \text{ for } 0 < \arg z < \pi \end{align}
For the modified Bessel functions, Hankel developed asymptotic expansions as well:

I_\alpha(z) \sim \frac{e^z}{\sqrt{2\pi z}} \left(1  \frac{4 \alpha^{2}  1}{8 z} + \frac{(4 \alpha^{2}  1) (4 \alpha^{2}  9)}{2! (8 z)^{2}}  \frac{(4 \alpha^{2}  1) (4 \alpha^{2}  9) (4 \alpha^{2}  25)}{3! (8 z)^{3}} + \cdots \right)\text{ for }\arg z<\tfrac{\pi}{2},^{[31]}

K_\alpha(z) \sim \sqrt{\frac{\pi}{2z}} e^{z} \left(1 + \frac{4 \alpha^{2}  1}{8 z} + \frac{(4 \alpha^{2}  1) (4 \alpha^{2}  9)}{2! (8 z)^{2}} + \frac{(4 \alpha^{2}  1) (4 \alpha^{2}  9) (4 \alpha^{2}  25)}{3! (8 z)^{3}} + \cdots \right)\text{ for }\arg z<\tfrac{3\pi}{2}.^{[32]}
When α = 1/2 all the terms except the first vanish and we have

\begin{align} I_{\frac{1}{2}}(z) &= \sqrt{\frac{2}{\pi z}}\sinh(z) \sim \frac{e^z}{\sqrt{2\pi z}} && \text{ for }\arg z<\tfrac{\pi}{2}, \\ K_{\frac{1}{2}}(z) &= \sqrt{\frac{\pi}{2z}} e^{z} \end{align}
For small arguments 0 < z \ll \sqrt{\alpha + 1}, we have:

I_\alpha(z) \sim \frac{1}{\Gamma(\alpha+1)} \left( \frac{z}{2} \right) ^\alpha

K_\alpha(z) \sim \begin{cases}  \ln \left (\frac{z}{2} \right )  \gamma & \text{if } \alpha=0 \\ \\ \frac{\Gamma(\alpha)}{2} \left( \frac{2}{z} \right) ^\alpha & \text{if } \alpha > 0. \end{cases}
Properties
For integer order α = n, J_{n} is often defined via a Laurent series for a generating function:

e^{(\frac{x}{2})(t1/t)} = \sum_{n=\infty}^\infty J_n(x) t^n,\!
an approach used by P. A. Hansen in 1843. (This can be generalized to noninteger order by contour integration or other methods.) Another important relation for integer orders is the Jacobi–Anger expansion:

e^{iz \cos(\phi)} = \sum_{n=\infty}^\infty i^n J_n(z) e^{in\phi},\!
and

e^{\pm iz \sin(\phi)} = J_0(z)+2\sum_{n=1}^\infty J_{2n}(z) \cos(2n\phi) \pm 2i \sum_{n=0}^\infty J_{2n+1}(z)\sin([2n+1]\phi),\!
which is used to expand a plane wave as a sum of cylindrical waves, or to find the Fourier series of a tonemodulated FM signal.
More generally, a series

f(z)=a_0^\nu J_\nu (z)+ 2 \cdot \sum_{k=1} a_k^\nu J_{\nu+k}(z)\!
is called Neumann expansion of ƒ. The coefficients for ν = 0 have the explicit form

a_k^0=\frac{1}{2 \pi i} \int_{z=c} f(z) O_k(z) \,dz,\!
where O_{k} is Neumann's polynomial.^{[33]}
Selected functions admit the special representation

f(z)=\sum_{k=0} a_k^\nu J_{\nu+2k}(z)\!
with

a_k^\nu=2(\nu+2k) \int_0^\infty f(z) \frac{J_{\nu+2k}(z)}z \,dz\!
due to the orthogonality relation

\int_0^\infty J_\alpha(z) J_\beta(z) \frac {dz} z= \frac 2 \pi \frac{\sin\left(\frac \pi 2 (\alpha\beta) \right)}{\alpha^2 \beta^2}.
More generally, if ƒ has a branchpoint near the origin of such a nature that

f(z)= \sum_{k=0} a_k J_{\nu+k}(z),
then

\mathcal{L} \left\{\sum_{k=0} a_k J_{\nu+k} \right\}(s)= \frac{1}{\sqrt{1+s^2}} \sum_{k=0} \frac{a_k}{(s+\sqrt{1+s^2})^{\nu+k}}
or

\sum_{k=0} a_k \xi^{\nu+k}= \frac{1+\xi^2}{2\xi} \mathcal L \{f \} \left( \frac{1\xi^2}{2\xi} \right),
where \mathcal L \{f \} is f's Laplace transform.^{[34]}
Another way to define the Bessel functions is the Poisson representation formula and the MehlerSonine formula:

\begin{align}J_\nu(z) &= \frac{ (\frac{z}{2})^\nu }{ \Gamma(\nu + \frac{1}{2} ) \sqrt{\pi} } \int_{1}^{1} e^{izs}(1  s^2)^{\nu  \frac{1}{2} } \,ds, \\ &=\frac 2 \,du,\end{align}
where ν > −1/2 and z ∈ C.^{[35]} This formula is useful especially when working with Fourier transforms.
The functions J_{α}, Y_{α}, H_{α}^{(1)}, and H_{α}^{(2)} all satisfy the recurrence relations:^{[36]}

\frac{2\alpha}{x} Z_\alpha(x) = Z_{\alpha1}(x) + Z_{\alpha+1}(x)\!

2\frac{dZ_\alpha}{dx} = Z_{\alpha1}(x)  Z_{\alpha+1}(x)\!
where Z denotes J, Y, H^{(1)}, or H^{(2)}. (These two identities are often combined, e.g. added or subtracted, to yield various other relations.) In this way, for example, one can compute Bessel functions of higher orders (or higher derivatives) given the values at lower orders (or lower derivatives). In particular, it follows that:^{[37]}

\left( \frac{1}{x} \frac{d}{dx} \right)^m \left[ x^\alpha Z_{\alpha} (x) \right] = x^{\alpha  m} Z_{\alpha  m} (x),

\left( \frac{1}{x} \frac{d}{dx} \right)^m \left[ \frac{Z_\alpha (x)}{x^\alpha} \right] = (1)^m \frac{Z_{\alpha + m} (x)}{x^{\alpha + m}}.
Modified Bessel functions follow similar relations :

e^{(\frac{x}{2})(t+1/t)} = \sum_{n=\infty}^\infty I_n(x) t^n,\!
and

e^{z \cos( \theta)} = I_0(z) + 2\sum_{n=1}^\infty I_n(z) \cos(n\theta).\!
The recurrence relation reads

C_{\alpha1}(x)  C_{\alpha+1}(x) = \frac{2\alpha}{x} C_\alpha(x)\!

C_{\alpha1}(x) + C_{\alpha+1}(x) = 2\frac{dC_\alpha}{dx}\!
where C_{α} denotes I_{α} or e^{απi}K_{α}. These recurrence relations are useful for discrete diffusion problems.
Because Bessel's equation becomes Hermitian (selfadjoint) if it is divided by x, the solutions must satisfy an orthogonality relationship for appropriate boundary conditions. In particular, it follows that:

\int_0^1 x J_\alpha(x u_{\alpha,m}) J_\alpha(x u_{\alpha,n}) \,dx = \frac{\delta_{m,n}}{2} [J_{\alpha+1}(u_{\alpha,m})]^2 = \frac{\delta_{m,n}}{2} [J_{\alpha}'(u_{\alpha,m})]^2,\!
where α > −1, δ_{m,n} is the Kronecker delta, and u_{α, m} is the mth zero of J_{α}(x). This orthogonality relation can then be used to extract the coefficients in the Fourier–Bessel series, where a function is expanded in the basis of the functions J_{α}(x u_{α, m}) for fixed α and varying m.
An analogous relationship for the spherical Bessel functions follows immediately:

\int_0^1 x^2 j_\alpha(x u_{\alpha,m}) j_\alpha(x u_{\alpha,n}) \,dx = \frac{\delta_{m,n}}{2} [j_{\alpha+1}(u_{\alpha,m})]^2.\!
If one defines a boxcar function of x that depends on a small parameter ε as:

f_\epsilon(x)=\epsilon\ \mathrm{rect}\left(\frac{x1}\epsilon\right)
(where rect() is the rectangle function) then the Hankel transform of it (of any given order α greater than −1/2), g_{ε}(k), approaches J_{α}(k) as ε approaches zero, for any given k. Conversely, the Hankel transform (of the same order) of g_{ε}(k) is f_{ε}(x):

\int_0^\infty k J_\alpha(kx) g_\epsilon(k) dk = f_\epsilon(x)
which is zero everywhere except near 1. As ε approaches zero, the righthand side approaches δ(x−1), where δ is the Dirac delta function. So by abuse of language (or "formally"), one says that

\int_0^\infty k J_\alpha(kx) J_\alpha(k) dk = \delta(x1)
even though the integral on the left is not actually defined. A change of variables then yields the closure equation:^{[38]}

\int_0^\infty x J_\alpha(ux) J_\alpha(vx) \,dx = \frac{1}{u} \delta(u  v)\!
for α > −1/2. The Hankel transform can express a fairly arbitrary function as an integral of Bessel functions of different scales. For the spherical Bessel functions the orthogonality relation is:

\int_0^\infty x^2 j_\alpha(ux) j_\alpha(vx) \,dx = \frac{\pi}{2u^2} \delta(u  v)\!
for α > −1. Again, this is a useful formal equation whose lefthand side is not actually defined.
Another important property of Bessel's equations, which follows from Abel's identity, involves the Wronskian of the solutions:

A_\alpha(x) \frac{dB_\alpha}{dx}  \frac{dA_\alpha}{dx} B_\alpha(x) = \frac{C_\alpha}{x},\!
where A_{α} and B_{α} are any two solutions of Bessel's equation, and C_{α} is a constant independent of x (which depends on α and on the particular Bessel functions considered). In particular,

J_\alpha(x) \frac{dY_\alpha}{dx}  \frac{dJ_\alpha}{dx} Y_\alpha(x) = \frac{2}{\pi x},\!
and

I_\alpha(x) \frac{dK_\alpha}{dx}  \frac{dI_\alpha}{dx} K_\alpha(x) = \frac{1}{x}.\!
(There are a large number of other known integrals and identities that are not reproduced here, but which can be found in the references.)
Multiplication theorem
The Bessel functions obey a multiplication theorem

\lambda^{\nu} J_\nu (\lambda z) = \sum_{n=0}^\infty \frac{1}{n!} \left(\frac{(1\lambda^2)z}{2}\right)^n J_{\nu+n}(z)
where λ and ν may be taken as arbitrary complex numbers, see.^{[39]}^{[40]} The above expression also holds if J is replaced by Y. The analogous identities for modified Bessel functions are

\lambda^{\nu} I_\nu (\lambda z) = \sum_{n=0}^\infty \frac{1}{n!} \left(\frac{(\lambda^21)z}{2}\right)^n I_{\nu+n}(z)
and

\lambda^{\nu} K_\nu (\lambda z) = \sum_{n=0}^\infty \frac{(1)^n}{n!} \left(\frac{(\lambda^21)z}{2}\right)^n K_{\nu+n}(z).
Bourget's hypothesis
Bessel himself originally proved that for nonnegative integers n, the equation J_{n}(x) = 0 has an infinite number of solutions in x.^{[41]} When the functions J_{n}(x) are plotted on the same graph, though, none of the zeros seem to coincide for different values of n except for the zero at x = 0. This phenomenon is known as Bourget's hypothesis after the nineteenth century French mathematician who studied Bessel functions. Specifically it states that for any integers n ≥ 0 and m ≥ 1, the functions J_{n}(x) and J_{n+m}(x) have no common zeros other than the one at x = 0. The hypothesis was proved by Carl Ludwig Siegel in 1929.^{[42]}
Selected identities^{[43]}

\begin{align} K_\frac{1}{2} (z) &= \sqrt{\frac{\pi}{2}} e^{z} z^{\tfrac{1}{2}}, \qquad z>0 \\ I_{\frac{1}{2}}(z) &= \sqrt{\frac{2}{\pi z}}\cosh(z) \\ I_{ \frac{1}{2}}(z) &= \sqrt{\frac{2}{\pi z}}\sinh(z) \\ I_\nu(z) &= \sum_{k=0} \frac{z^k}{k!} J_{\nu+k}(z) \\ J_\nu(z) &= \sum_{k=0} (1)^k \frac{z^k}{k!} I_{\nu+k}(z) \\ I_\nu (\lambda z) &= \lambda^\nu \sum_{k=0} \frac{\left((\lambda^21)\frac z 2\right)^k}{k!} I_{\nu+k}(z) \\ I_\nu (z_1+z_2) &= \sum_{k=\infty}^\infty I_{\nuk}(z_1)I_k(z_2) \\ J_\nu (z_1\pm z_2) &= \sum_{k=\infty}^\infty J_{\nu \mp k}(z_1)J_k(z_2) \\ I_\nu (z) &= \tfrac{z}{2 \nu} \left (I_{\nu1}(z)I_{\nu+1}(z) \right ) \\ J_\nu (z) &= \tfrac{z}{2 \nu} \left (J_{\nu1}(z)+J_{\nu+1}(z) \right ) \\ J_\nu'(z) &= \begin{cases}\tfrac{1}{2} \left (J_{\nu1}(z)J_{\nu+1}(z) \right) & \nu \neq 0 \\ J_1(z) & \nu =0 \end{cases} \\ I_\nu'(z) &= \begin{cases}\tfrac{1}{2} \left (I_{\nu1}(z)+I_{\nu+1}(z) \right) & \nu \neq 0 \\ I_1(z) & \nu =0 \end{cases} \\ \left(\tfrac{z}{2}\right)^\nu &= \Gamma(\nu) \sum_{k=0} I_{\nu+2k}(z)(\nu+2k){\nu\choose k} = \Gamma(\nu) \sum_{k=0}(1)^k J_{\nu+2k}(z)(\nu+2k){\nu \choose k} = \Gamma(\nu+1) \sum_{k=0}\frac{\left(\tfrac{z}{2}\right)^k}{k!} J_{\nu+k}(z)\\ 1 &= \sum_{n=0}^\infty (2n+1) j_n(z)^2\\ \frac{\sin(2z)}{2z} &= \sum_{n=0}^\infty (1)^n (2n+1) j_n(z)^2 \end{align}
See also
Notes

^ ^{a} ^{b} Abramowitz and Stegun, p. 360, 9.1.10.

^ Abramowitz and Stegun, p. 358, 9.1.5.

^ ^{a} ^{b} ^{c}

^ Watson, p. 176

^ http://www.math.ohiostate.edu/~gerlach/math/BVtypset/node122.html

^ http://www.nbi.dk/~polesen/borel/node15.html

^ Arfken & Weber, exercise 11.1.17.

^ Abramowitz and Stegun, p. 362, 9.1.69.

^ Szegö, G. Orthogonal Polynomials, 4th ed. Providence, RI: Amer. Math. Soc., 1975.

^ http://www.mhtlab.uwaterloo.ca/courses/me755/web_chap4.pdf

^ Watson, p. 178.

^ Abramowitz and Stegun, p. 358, 9.1.3, 9.1.4.

^ Abramowitz and Stegun, p. 358, 9.1.6.

^ Abramowitz and Stegun, p. 360, 9.1.25.

^ Watson, p. 178

^ Abramowitz and Stegun, p. 375, 9.6.2, 9.6.10, 9.6.11.

^ Abramowitz and Stegun, p. 374, 9.6.1.

^ Quantum electrodynamics. Greiner, Walter and Reinhardt, Joachim. 2009 Springer. pg. 72

^ Watson, p. 181.

^ M.Kh.Khokonov. Cascade Processes of Energy Loss by Emission of Hard Photons, JETP, V.99, No.4, pp. 690707 (2004). Derived from formulas sourced to I. S. Gradshteĭn and I. M. Ryzhik, Table of Integrals, Series, and Products (Fizmatgiz, Moscow, 1963; Academic, New York, 1980).

^ Referred to as such in: Teichroew, D. The Mixture of Normal Distributions with Different Variances, The Annals of Mathematical Statistics. Vol. 28, No. 2 (Jun., 1957), pp. 510–512

^ Abramowitz and Stegun, p. 437, 10.1.1.

^ Abramowitz and Stegun, p. 439, 10.1.25, 10.1.26;

^ Abramowitz and Stegun, p. 438, 10.1.11.

^ Abramowitz and Stegun, p. 438, 10.1.12;

^ Abramowitz and Stegun, p. 439, 10.1.39.

^ Abramowitz and Stegun, p. 439, 10.1.23, 10.1.24.

^ Hong Du, "Miescattering calculation," Applied Optics 43 (9), 1951–1956 (2004)

^ Abramowitz and Stegun, p. 364, 9.2.1;

^ NIST Digital Library of Mathematical Functions, Section 10.11.

^ Abramowitz and Stegun, p. 377, 9.7.1;

^ Abramowitz and Stegun, p. 378, 9.7.2;

^ Abramowitz and Stegun, p. 363, 9.1.82 ff.

^ E. T. Whittaker, G. N. Watson, A course in modern Analysis p. 536

^ I.S. Gradshteyn (И.С. Градштейн), I.M. Ryzhik (И.М. Рыжик); Alan Jeffrey, Daniel Zwillinger, editors. Table of Integrals, Series, and Products, seventh edition. Academic Press, 2007. ISBN 9780123736376. Equation 8.411.10

^ Abramowitz and Stegun, p. 361, 9.1.27.

^ Abramowitz and Stegun, p. 361, 9.1.30.

^ Arfken & Weber, section 11.2

^ Abramowitz and Stegun, p. 363, 9.1.74.

^ C. Truesdell, "On the Addition and Multiplication Theorems for the Special Functions", Proceedings of the National Academy of Sciences, Mathematics, (1950) pp.752–757.

^ F. Bessel, Untersuchung des Theils der planetarischen Störungen, Berlin Abhandlungen (1824), article 14.

^ Watson, pp. 484–5

^ See, for example, Lide DR. CRC handbook of chemistry and physics: a readyreference book of chemical CRC Press, 2004, ISBN 0849304857, p. A95
References

See also chapter 10.

Arfken, George B. and Hans J. Weber, Mathematical Methods for Physicists, 6th edition (Harcourt: San Diego, 2005). ISBN 0120598760.

Bayin, S.S. Mathematical Methods in Science and Engineering, Wiley, 2006, Chapter 6.

Bayin, S.S., Essentials of Mathematical Methods in Science and Engineering, Wiley, 2008, Chapter 11.

Bowman, Frank Introduction to Bessel Functions (Dover: New York, 1958). ISBN 0486604624.

G. Mie, "Beiträge zur Optik trüber Medien, speziell kolloidaler Metallösungen", Ann. Phys. Leipzig 25 (1908), p. 377.


B Spain, M.G. Smith, Functions of mathematical physics, Van Nostrand Reinhold Company, London, 1970. Chapter 9 deals with Bessel functions.

N. M. Temme, Special Functions. An Introduction to the Classical Functions of Mathematical Physics, John Wiley and Sons, Inc., New York, 1996. ISBN 0471113131. Chapter 9 deals with Bessel functions.

Watson, G.N., A Treatise on the Theory of Bessel Functions, Second Edition, (1995) Cambridge University Press. ISBN 0521483913.

External links




Wolfram function pages on Bessel J and Y functions, and modified Bessel I and K functions. Pages include formulas, function evaluators, and plotting calculators.

Wolfram Mathworld – Bessel functions of the first kind

Bessel functions _{ν}J, _{ν}Y, _{ν}I and _{ν}K in Librow Function handbook.

F. W. J. Olver, L. C. Maximon, Bessel Functions (chapter 10 of the Digital Library of Mathematical Functions).
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