This work presents a theoretical study on the analytical calculation of the lineshape of polarization spectroscopy (PS) for the transition line 5
_{s}
^{2}
^{1}
S
_{0}
→ 5
_{s}
5
_{p}
^{1}
P
_{1}
of
^{88}
Sr. From the obtained analytical form of the PS spectrum, we were able to identify how the saturation affected the lineshape of the PS spectrum. The results obtained will be useful for polarization spectroscopy experiments using the alkalineearth atoms such as Sr or Yb.
I. INTRODUCTION
Due to the ability to provide a dispersive spectroscopic lineshape, polarization spectroscopy (PS)
[1]
has been widely used and studied in particular for laser frequency stabilization. In PS, a circular birefringence is established by a circularly polarized pump beam. This is detected by measuring the rotation angle of a linearly polarized probe beam propagating in the opposite direction to the pump beam. The subDoppler feature originates from the fact that only the atoms belonging to certain velocity classes can experience the pump and probe beams simultaneously. The atoms with zero velocity contribute to the resonance signals, whereas the crossover signals result from the contribution from the atoms satisfying the condition that the frequency spacing of the excited state is equal to twice the Doppler shift.
PS has been realized for many kinds of atoms such as Li
[2]
, Rb
[3

6]
, Cs
[6
,
7]
, K
[8]
, He
[9]
, and Sr
[10]
. In the case of all the atoms except for Sr, the PS spectra result from three operating mechanisms such as Zeeman and hyperfine optical pumping and the saturation effect. In contrast, the PS for Sr results from only the saturation effect because there are no degenerate sublevels in the ground state. Since the isotopes
^{84}
Sr,
^{86}
Sr, and
^{88}
Sr possess zero nuclear spin (
I
= 0), whereas
^{87}
Sr possesses
I
= 9/2, the
J_{g}
= 0 →
J_{e}
= 1 transition exists in the isotopes
^{84}
Sr,
^{86}
Sr, and
^{88}
Sr. In this paper, we will consider
^{88}
Sr. In addition, Yb isotopes with mass numbers, 168, 170, 172, 174, and 176, also possess zero nuclear spin. Because the energy level structure of Sr (and Yb) is very simple, it is possible to obtain exact analytical solutions for the PS spectra. The analytical solution of saturated absorption spectroscopy (SAS) for the ideal twolevel atoms was presented in the textbook
[11]
. Also, SAS
[12]
and PS
[13]
for Rb atoms were analytically studied in the low intensity limit. In this paper, we present analytical solutions of PS for the transition
J_{g}
=0→
J_{e}
=1 of Sr (or Yb) atoms where the intensity of the pump beam is arbitrary. This paper is organized as follows. Section II describes the theory of calculating analytical lineshape in PS. Results and discussion are presented in Sec. III. The final section summarizes the results of the paper.
II. THEORY
The energy level diagram for the transition
J_{g}
=0→
J_{e}
=1 of an atom (
^{88}
Sr or Yb) is shown in
Fig. 1
. The ground state is 
g
>, while three degenerate excited states are 
e
_{−}
>, 
e
_{0}
>, and 
e
_{+}
> where magnetic quantum numbers are 1, 0, and 1, respectively. The pump beam of
σ
^{+}
polarization excites the transition from 
g
> to 
e
_{+}
>, whereas the linearly polarized probe beam excites both the transitions from 
e
> to 
e
_{±}
>.
ω
_{0}
is the resonance frequency, λ is the wavelength,
k
= 2
π/λ
is the wave vector, Ω
_{1(2)}
are the Rabi frequencies for the pump (probe) beam,
Γ
is the
Energy level diagram for the transition 5s^{2 1}s_{0} → 5s5p ^{1}P_{1} in the absence of an external magnetic field.
decay rate of the excited state, and
γ
_{t}
is the decay rate of the optical coherence which is equal to
Г
/2 if there is no dephasing mechanism. The laser frequencies of the pump and probe beams felt by an atom moving at velocity,
v
, are
ω
_{1}
=
ω
+
kv
and
ω
_{2}
=
ω
−
kv
, respectively.
Then, the susceptibilities of the
σ
^{±}
components of the probe beam for an atom moving at velocity,
v
, are given by
[14]
where
p
denotes the population of the ground state,
q
± denotes the populations of the excited states, 
e
_{±}
>, and
N
_{at}
represents the atomic density. The populations in Eq. (1) are calculated analytically by considering the effect of only the pump beam. Since the
σ
^{+}
polarized pump laser field couples only the ground state and the excited state (
e
_{±}
>), we can use the results for the case of a twolevel atom. Thus, we refer to our previous result
[14]
or a textbook
[15]
, and the results are given by
and
q
_{0}
=
q
_{−}
= 0, where
A
= (
ω
_{1}

ω
_{0}
)
^{2}
+
γ_{t}
^{2}
and
B
=Ω
_{1}
^{2}
γ_{t}
/Γ.
Therefore, the susceptibilities in Eq. (1) become the following equations:
Equations (2) and (3) are then averaged over the Maxwell Boltzmann velocity distribution a
where
u
is the most probable speed of the atom. Equation (4) is further simplified by changing the integration variable as
where
and
δ
(=
ω
−
ω
_{0}
) is the detuning and
s
_{0}
(=Ω
_{1}
^{2}
/
γ
_{t}
Γ)=
I
_{1}
/
I_{s}
is the onresonance saturation parameter where
I
_{1}
is the pump beam intensity and
I_{s}
=
πhc
Γ/(3
λ
^{3}
) is the saturation intensity with
c
being the speed of light in vacuum. The integration in Eq. (5) can be easily performed using a convolution theorem. When
γ
_{t}
≪
ku
, the real and imaginary parts of the susceptibilities are given by
respectively.
In PS, a linearly polarized probe beam (intensity is
I
_{0}
and polarization vector is
is incident on an atomic cell of length
l
along the
z
axis. After traversing the cell, the polarization of the probe beam changes due to the circular anisotropy from the pump beam. The electric field of the probe beam is then given by
[5
,
14]
where
E
_{0}
is the amplitude of the incident probe beam’s electric field,
a
_{±}
=
e
^{(k/2)χi±l}
, and
n
_{±}
≅ 1+(
χ
_{±}
/2) are the refractive indices of the
σ
^{±}
components of the probe beam.
are the spherical bases where
are the unit vectors for
x
and
y
axes, respectively. The inclination angle of the electric field in Eq. (6) with respect to the
x
axis is given by
θ
+
ς
where
θ
is the inclination angle of the incident probe beam’s polarization and
ς
=(
kl
/2)(
n
_{}

n
_{+}
) ≅ (
kl
/4)(
χ
_{}
^{r}

χ
_{+}
^{r}
)is the rotation angle of the probe beam's polarization after traversing the atomic cell
[16]
. Then, the difference in the intensities along the
x
and
y
axes, Δ
I
=
I_{x}
−
I_{y}
, is given by
and becomes further
when
θ
=
π
/4. Since the rotation angle,
ς
, is very small, the PS signal is given by
where
is the average of the absorption coefficients. The difference in the real parts of the susceptibilities (Δ
χ^{r}
≡
χ_{−}^{r}−χ_{+}^{r}
) is given by
where
(a) Typical calculated PS spectra for several pump beam intensities. (b) Dependence of the amplitude and the magnitude of the slope on the onresonance saturation parameter.
We neglect
e
^{−δ2/(ku)2}
in Eq. (8) because 
δ
 ≪
ku
.
III. RESULTS AND DISCUSSION
The typical PS spectra (Δ
χ^{r}
) for several pump beam intensities are presented in
Fig. 2
(a). In
Fig. 2
(a), the saturation parameters were
s
_{0}
= 1, 5, 10, 50, and 100. The saturation parameter of
s
_{0}
= 100 corresponds to the intensities of 4.27 W/cm
^{2}
because the saturation intensity of Sr atom is about 4.27×10
^{2}
W/cm
^{2}
. The amplitude of the spectrum, defined as Δ
χ^{r}
 at
x
=±1, and accordingly at the detunings of
is given by
and the magnitude of the slope of the PS spectrum at the resonance condition is given by
The calculated amplitude and slope as functions of
s
_{0}
are presented in
Fig. 2
(b). In
Fig. 2
(b), the amplitude increases and is then saturated at the value of
C
_{0}
/4. In
Fig. 2
(b), the slope is maximum when
This value corresponds to the intensity of 0.206 W/cm
^{2}
. This is in excellent agreement with the experimental results in Fig. 4(b) in Ref.
[10]
.
IV. CONCLUSION
In this paper we have presented a theoretical study of lineshape in PS for the transition
J_{g}
=0→
J_{e}
=1 of Sr atoms. Equations (7) and (8) are the main result of the paper. The amplitude and the slope of the spectrum are presented in Eq. (9) and Eq. (10), respectively. The theoretical results were compared with experimental results presented in Ref.
[10]
, and excellent agreement between them was found. Since the obtained results in this paper are very concise, these can be applied to study of PS for other atoms such as Yb and to study of other spectroscopy such as subDoppler dichroic atomic vapor laser lock (DAVLL)
[10]
.
Acknowledgements
This research was supported by Basic Science Research Program through the National Research Foundation of Korea(NRF) funded by the Ministry of Education, Science and Technology(20110009886).
Ohtsubo N.
,
Aoki T.
,
Torii Y.
(2012)
“Buffergasassisted polarization spectroscopy of6Li”
Opt. Lett.
37
2865 
2867
DOI : 10.1364/OL.37.002865
Pearman C. P.
,
Adams C. S.
,
Cox S. G.
,
Griffin P. F.
,
Smith D. A.
,
Hughes I. G.
(2002)
“Polarization spectroscopy of a closed atomic transition: applications to laser frequency locking”
J. Phys. B
35
5141 
5151
DOI : 10.1088/09534075/35/24/315
Yoshikawa Y.
,
Umeki T.
,
Mukae T.
,
Torii Y.
,
Kuga T.
(2003)
“Frequency stabilization of a laser diode with use of lightinduced birefringence in an atomic vapor”
Appl. Opt.
42
6645 
6649
DOI : 10.1364/AO.42.006645
Do H. D.
,
Moon G.
,
Noh H. R.
(2008)
“Polarization spectroscopy of rubidium atoms: theory and experiment”
Phys. Rev. A
77
032513 
DOI : 10.1103/PhysRevA.77.032513
Harris M. L.
,
Adams C. S.
,
Cornish S. L.
,
McLeod I. C.
,
Tarleton E.
,
Hughes I. G.
(2006)
“Polarization spectroscopy in rubidium and cesium”
Phys. Rev. A
73
062509 
DOI : 10.1103/PhysRevA.73.062509
Carr C.
,
Adams C. S.
,
Weatherill K. J.
(2012)
“Polarization spectroscopy of an excited state transition”
Opt. Lett.
37
118 
120
DOI : 10.1364/OL.37.000118
Pahwa K.
,
Mudarikwa L.
,
Goldwin J.
(2012)
“Polarization spectroscopy and magneticallyinduced dichroism of the potassium D2 lines”
Opt. Express
20
17456 
17466
DOI : 10.1364/OE.20.017456
Wu T.
,
Peng X.
,
Gong W.
,
Zhan Y.
,
Lin Z.
,
Luo B.
,
Guo H.
(2013)
“Observation and optimization of 4He atomic polarization spectroscopy”
Opt. Lett.
38
986 
988
DOI : 10.1364/OL.38.000986
Javaux C.
,
Hughes I. G.
,
Locheada G.
,
Millen J.
,
Jones M. P. A.
(2010)
“Modulationfree pumpprobe spectroscopy of strontium atoms”
Eur. Phys. J. D
57
151 
154
DOI : 10.1140/epjd/e2010000294
Foot C. J.
2005
Atomic Physics
Oxford University Press
New York, USA
Moon G.
,
Noh H. R.
(2008)
“Analytic solutions for the saturated absorption spectra”
J. Opt. Soc. Am
25
701 
711
Do H. D.
,
Heo M. S.
,
Moon G.
,
Noh H. R.
,
Jhe W.
(2008)
“Analytic calculation of the lineshapes in polarization spectroscopy of rubidium”
Opt. Commun.
281
4042 
4047
DOI : 10.1016/j.optcom.2008.04.022
Noh H. R.
(2009)
“Effect of optical pumping in saturated absorption spectroscopy: an analytic study for twolevel atoms”
Eur. J. Phys.
30
1181 
1187
DOI : 10.1088/01430807/30/5/025
CohenTannoudji C.
,
DupontRoc J.
,
Grynberg G.
1992
Atomphoton Interactions, Basic Processes and Applications
Wiley
New York, USA
Seo M. J.
,
Won J. Y.
,
Noh H. R.
(2011)
“Variation in the polarization state of arbitrarily polarized light via a circular anisotropic atomic medium”
J. Korean Phys. Soc.
59
253 
256
DOI : 10.3938/jkps.59.253