- Source: Lamb shift
In physics, the Lamb shift, named after Willis Lamb, is an anomalous difference in energy between two electron orbitals in a hydrogen atom. The difference was not predicted by theory and it cannot be derived from the Dirac equation, which predicts identical energies. Hence the Lamb shift is a deviation from theory seen in the differing energies contained by the 2S1/2 and 2P1/2 orbitals of the hydrogen atom.
The Lamb shift is caused by interactions between the virtual photons created through vacuum energy fluctuations and the electron as it moves around the hydrogen nucleus in each of these two orbitals. The Lamb shift has since played a significant role through vacuum energy fluctuations in theoretical prediction of Hawking radiation from black holes.
This effect was first measured in 1947 in the Lamb–Retherford experiment on the hydrogen microwave spectrum and this measurement provided the stimulus for renormalization theory to handle the divergences. It was the harbinger of modern quantum electrodynamics developed by Julian Schwinger, Richard Feynman, Ernst Stueckelberg, Sin-Itiro Tomonaga and Freeman Dyson. Lamb won the Nobel Prize in Physics in 1955 for his discoveries related to the Lamb shift.
Importance
In 1978, on Lamb's 65th birthday, Freeman Dyson addressed him as follows: "Those years, when the Lamb shift was the central theme of physics, were golden years for all the physicists of my generation. You were the first to see that this tiny shift, so elusive and hard to measure, would clarify our thinking about particles and fields."
Derivation
This heuristic derivation of the electrodynamic level shift follows Theodore A. Welton's approach.
The fluctuations in the electric and magnetic fields associated with the QED vacuum perturbs the electric potential due to the atomic nucleus. This perturbation causes a fluctuation in the position of the electron, which explains the energy shift. The difference of potential energy is given by
Δ
V
=
V
(
r
→
+
δ
r
→
)
−
V
(
r
→
)
=
δ
r
→
⋅
∇
V
(
r
→
)
+
1
2
(
δ
r
→
⋅
∇
)
2
V
(
r
→
)
+
⋯
{\displaystyle \Delta V=V({\vec {r}}+\delta {\vec {r}})-V({\vec {r}})=\delta {\vec {r}}\cdot \nabla V({\vec {r}})+{\frac {1}{2}}(\delta {\vec {r}}\cdot \nabla )^{2}V({\vec {r}})+\cdots }
Since the fluctuations are isotropic,
⟨
δ
r
→
⟩
v
a
c
=
0
,
{\displaystyle \langle \delta {\vec {r}}\rangle _{\rm {vac}}=0,}
⟨
(
δ
r
→
⋅
∇
)
2
⟩
v
a
c
=
1
3
⟨
(
δ
r
→
)
2
⟩
v
a
c
∇
2
.
{\displaystyle \langle (\delta {\vec {r}}\cdot \nabla )^{2}\rangle _{\rm {vac}}={\frac {1}{3}}\langle (\delta {\vec {r}})^{2}\rangle _{\rm {vac}}\nabla ^{2}.}
So one can obtain
⟨
Δ
V
⟩
=
1
6
⟨
(
δ
r
→
)
2
⟩
v
a
c
⟨
∇
2
(
−
e
2
4
π
ϵ
0
r
)
⟩
a
t
.
{\displaystyle \langle \Delta V\rangle ={\frac {1}{6}}\langle (\delta {\vec {r}})^{2}\rangle _{\rm {vac}}\left\langle \nabla ^{2}\left({\frac {-e^{2}}{4\pi \epsilon _{0}r}}\right)\right\rangle _{\rm {at}}.}
The classical equation of motion for the electron displacement (δr)k→ induced by a single mode of the field of wave vector k→ and frequency ν is
m
d
2
d
t
2
(
δ
r
)
k
→
=
−
e
E
k
→
,
{\displaystyle m{\frac {d^{2}}{dt^{2}}}(\delta r)_{\vec {k}}=-eE_{\vec {k}},}
and this is valid only when the frequency ν is greater than ν0 in the Bohr orbit,
ν
>
π
c
/
a
0
{\displaystyle \nu >\pi c/a_{0}}
. The electron is unable to respond to the fluctuating field if the fluctuations are smaller than the natural orbital frequency in the atom.
For the field oscillating at ν,
δ
r
(
t
)
≅
δ
r
(
0
)
(
e
−
i
ν
t
+
e
i
ν
t
)
,
{\displaystyle \delta r(t)\cong \delta r(0)(e^{-i\nu t}+e^{i\nu t}),}
therefore
(
δ
r
)
k
→
≅
e
m
c
2
k
2
E
k
→
=
e
m
c
2
k
2
E
k
→
(
a
k
→
e
−
i
ν
t
+
i
k
→
⋅
r
→
+
h
.
c
.
)
with
E
k
→
=
(
ℏ
c
k
/
2
ϵ
0
Ω
)
1
/
2
,
{\displaystyle (\delta r)_{\vec {k}}\cong {\frac {e}{mc^{2}k^{2}}}E_{\vec {k}}={\frac {e}{mc^{2}k^{2}}}{\mathcal {E}}_{\vec {k}}\left(a_{\vec {k}}e^{-i\nu t+i{\vec {k}}\cdot {\vec {r}}}+h.c.\right)\qquad {\text{with}}\qquad {\mathcal {E}}_{\vec {k}}=\left({\frac {\hbar ck/2}{\epsilon _{0}\Omega }}\right)^{1/2},}
where
Ω
{\displaystyle \Omega }
is some large normalization volume (the volume of the hypothetical "box" containing the hydrogen atom), and
h
.
c
.
{\displaystyle h.c.}
denotes the hermitian conjugate of the preceding term. By the summation over all
k
→
,
{\displaystyle {\vec {k}},}
⟨
(
δ
r
→
)
2
⟩
v
a
c
=
∑
k
→
(
e
m
c
2
k
2
)
2
⟨
0
|
(
E
k
→
)
2
|
0
⟩
=
∑
k
→
(
e
m
c
2
k
2
)
2
(
ℏ
c
k
2
ϵ
0
Ω
)
=
2
Ω
(
2
π
)
3
4
π
∫
d
k
k
2
(
e
m
c
2
k
2
)
2
(
ℏ
c
k
2
ϵ
0
Ω
)
since continuity of
k
→
implies
∑
k
→
→
2
Ω
(
2
π
)
3
∫
d
3
k
=
1
2
ϵ
0
π
2
(
e
2
ℏ
c
)
(
ℏ
m
c
)
2
∫
d
k
k
{\displaystyle {\begin{aligned}\langle (\delta {\vec {r}})^{2}\rangle _{\rm {vac}}&=\sum _{\vec {k}}\left({\frac {e}{mc^{2}k^{2}}}\right)^{2}\left\langle 0\left|(E_{\vec {k}})^{2}\right|0\right\rangle \\&=\sum _{\vec {k}}\left({\frac {e}{mc^{2}k^{2}}}\right)^{2}\left({\frac {\hbar ck}{2\epsilon _{0}\Omega }}\right)\\&=2{\frac {\Omega }{(2\pi )^{3}}}4\pi \int dkk^{2}\left({\frac {e}{mc^{2}k^{2}}}\right)^{2}\left({\frac {\hbar ck}{2\epsilon _{0}\Omega }}\right)&&{\text{since continuity of }}{\vec {k}}{\text{ implies }}\sum _{\vec {k}}\to 2{\frac {\Omega }{(2\pi )^{3}}}\int d^{3}k\\&={\frac {1}{2\epsilon _{0}\pi ^{2}}}\left({\frac {e^{2}}{\hbar c}}\right)\left({\frac {\hbar }{mc}}\right)^{2}\int {\frac {dk}{k}}\end{aligned}}}
This result diverges when no limits about the integral (at both large and small frequencies). As mentioned above, this method is expected to be valid only when
ν
>
π
c
/
a
0
{\displaystyle \nu >\pi c/a_{0}}
, or equivalently
k
>
π
/
a
0
{\displaystyle k>\pi /a_{0}}
. It is also valid only for wavelengths longer than the Compton wavelength, or equivalently
k
<
m
c
/
ℏ
{\displaystyle k
. Therefore, one can choose the upper and lower limit of the integral and these limits make the result converge.
⟨
(
δ
r
→
)
2
⟩
v
a
c
≅
1
2
ϵ
0
π
2
(
e
2
ℏ
c
)
(
ℏ
m
c
)
2
ln
4
ϵ
0
ℏ
c
e
2
{\displaystyle \langle (\delta {\vec {r}})^{2}\rangle _{\rm {vac}}\cong {\frac {1}{2\epsilon _{0}\pi ^{2}}}\left({\frac {e^{2}}{\hbar c}}\right)\left({\frac {\hbar }{mc}}\right)^{2}\ln {\frac {4\epsilon _{0}\hbar c}{e^{2}}}}
.
For the atomic orbital and the Coulomb potential,
⟨
∇
2
(
−
e
2
4
π
ϵ
0
r
)
⟩
a
t
=
−
e
2
4
π
ϵ
0
∫
d
r
→
ψ
∗
(
r
→
)
∇
2
(
1
r
)
ψ
(
r
→
)
=
e
2
ϵ
0
|
ψ
(
0
)
|
2
,
{\displaystyle \left\langle \nabla ^{2}\left({\frac {-e^{2}}{4\pi \epsilon _{0}r}}\right)\right\rangle _{\rm {at}}={\frac {-e^{2}}{4\pi \epsilon _{0}}}\int d{\vec {r}}\psi ^{*}({\vec {r}})\nabla ^{2}\left({\frac {1}{r}}\right)\psi ({\vec {r}})={\frac {e^{2}}{\epsilon _{0}}}|\psi (0)|^{2},}
since it is known that
∇
2
(
1
r
)
=
−
4
π
δ
(
r
→
)
.
{\displaystyle \nabla ^{2}\left({\frac {1}{r}}\right)=-4\pi \delta ({\vec {r}}).}
For p orbitals, the nonrelativistic wave function vanishes at the origin (at the nucleus), so there is no energy shift. But for s orbitals there is some finite value at the origin,
ψ
2
S
(
0
)
=
1
(
8
π
a
0
3
)
1
/
2
,
{\displaystyle \psi _{2S}(0)={\frac {1}{(8\pi a_{0}^{3})^{1/2}}},}
where the Bohr radius is
a
0
=
4
π
ϵ
0
ℏ
2
m
e
2
.
{\displaystyle a_{0}={\frac {4\pi \epsilon _{0}\hbar ^{2}}{me^{2}}}.}
Therefore,
⟨
∇
2
(
−
e
2
4
π
ϵ
0
r
)
⟩
a
t
=
e
2
ϵ
0
|
ψ
2
S
(
0
)
|
2
=
e
2
8
π
ϵ
0
a
0
3
{\displaystyle \left\langle \nabla ^{2}\left({\frac {-e^{2}}{4\pi \epsilon _{0}r}}\right)\right\rangle _{\rm {at}}={\frac {e^{2}}{\epsilon _{0}}}|\psi _{2S}(0)|^{2}={\frac {e^{2}}{8\pi \epsilon _{0}a_{0}^{3}}}}
.
Finally, the difference of the potential energy becomes:
⟨
Δ
V
⟩
=
4
3
e
2
4
π
ϵ
0
e
2
4
π
ϵ
0
ℏ
c
(
ℏ
m
c
)
2
1
8
π
a
0
3
ln
4
ϵ
0
ℏ
c
e
2
=
α
5
m
c
2
1
6
π
ln
1
π
α
,
{\displaystyle \langle \Delta V\rangle ={\frac {4}{3}}{\frac {e^{2}}{4\pi \epsilon _{0}}}{\frac {e^{2}}{4\pi \epsilon _{0}\hbar c}}\left({\frac {\hbar }{mc}}\right)^{2}{\frac {1}{8\pi a_{0}^{3}}}\ln {\frac {4\epsilon _{0}\hbar c}{e^{2}}}=\alpha ^{5}mc^{2}{\frac {1}{6\pi }}\ln {\frac {1}{\pi \alpha }},}
where
α
{\displaystyle \alpha }
is the fine-structure constant. This shift is about 500 MHz, within an order of magnitude of the observed shift of 1057 MHz. This is equal to an energy of only 7.00 x 10^-25 J., or 4.37 x 10^-6 eV.
Welton's heuristic derivation of the Lamb shift is similar to, but distinct from, the calculation of the Darwin term using Zitterbewegung, a contribution to the fine structure that is of lower order in
α
{\displaystyle \alpha }
than the Lamb shift.: 80–81
Lamb–Retherford experiment
In 1947 Willis Lamb and Robert Retherford carried out an experiment using microwave techniques to stimulate radio-frequency transitions between
2S1/2 and 2P1/2 levels of hydrogen. By using lower frequencies than for optical transitions the Doppler broadening could be neglected (Doppler broadening is proportional to the frequency). The energy difference Lamb and Retherford found was a rise of about 1000 MHz (0.03 cm−1) of the 2S1/2 level above the 2P1/2 level.
This particular difference is a one-loop effect of quantum electrodynamics, and can be interpreted as the influence of virtual photons that have been emitted and re-absorbed by the atom. In quantum electrodynamics the electromagnetic field is quantized and, like the harmonic oscillator in quantum mechanics, its lowest state is not zero. Thus, there exist small zero-point oscillations that cause the electron to execute rapid oscillatory motions. The electron is "smeared out" and each radius value is changed from r to r + δr (a small but finite perturbation).
The Coulomb potential is therefore perturbed by a small amount and the degeneracy of the two energy levels is removed. The new potential can be approximated (using atomic units) as follows:
⟨
E
p
o
t
⟩
=
−
Z
e
2
4
π
ϵ
0
⟨
1
r
+
δ
r
⟩
.
{\displaystyle \langle E_{\mathrm {pot} }\rangle =-{\frac {Ze^{2}}{4\pi \epsilon _{0}}}\left\langle {\frac {1}{r+\delta r}}\right\rangle .}
The Lamb shift itself is given by
Δ
E
L
a
m
b
=
α
5
m
e
c
2
k
(
n
,
0
)
4
n
3
f
o
r
ℓ
=
0
{\displaystyle \Delta E_{\mathrm {Lamb} }=\alpha ^{5}m_{e}c^{2}{\frac {k(n,0)}{4n^{3}}}\ \mathrm {for} \ \ell =0\,}
with k(n, 0) around 13 varying slightly with n, and
Δ
E
L
a
m
b
=
α
5
m
e
c
2
1
4
n
3
[
k
(
n
,
ℓ
)
±
1
π
(
j
+
1
2
)
(
ℓ
+
1
2
)
]
f
o
r
ℓ
≠
0
a
n
d
j
=
ℓ
±
1
2
,
{\displaystyle \Delta E_{\mathrm {Lamb} }=\alpha ^{5}m_{e}c^{2}{\frac {1}{4n^{3}}}\left[k(n,\ell )\pm {\frac {1}{\pi (j+{\frac {1}{2}})(\ell +{\frac {1}{2}})}}\right]\ \mathrm {for} \ \ell \neq 0\ \mathrm {and} \ j=\ell \pm {\frac {1}{2}},}
with log(k(n,ℓ)) a small number (approx. −0.05) making k(n,ℓ) close to unity.
For a derivation of ΔELamb see for example:
In the hydrogen spectrum
In 1947, Hans Bethe was the first to explain the Lamb shift in the hydrogen spectrum, and he thus laid the foundation for the modern development of quantum electrodynamics. Bethe was able to derive the Lamb shift by implementing the idea of mass renormalization, which allowed him to calculate the observed energy shift as the difference between the shift of a bound electron and the shift of a free electron.
The Lamb shift currently provides a measurement of the fine-structure constant α to better than one part in a million, allowing a precision test of quantum electrodynamics.
See also
Uehling potential, first approximation to the Lamb shift
Shelter Island Conference
Zeeman effect used to measure the Lamb shift
References
Further reading
Smirnov, Boris M. (2003). Physics of atoms and ions. Springer. pp. 39–41. ISBN 0-387-95550-X.
Scully, M.O.; Zubairy, M.S. (1997). "§1.3 Lamb shift". Quantum optics. Cambridge University Press. pp. 13–16. ISBN 0-521-43595-1.
External links
Hans Bethe talking about Lamb-shift calculations on Web of Stories
Nobel Prize biography of Willis Lamb
Nobel lecture of Willis Lamb: Fine Structure of the Hydrogen Atom
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